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Contents

Section 10.1 - Fields of Force

Section 10.2 - Voltage Related To Field

Section 10.3 - Fields by Superposition

Section 10.4 - Energy In Fields

Section 10.5 - LRC Circuits

Section 10.6 - Fields by Gauss' Law

Section 10.7 - Gauss' Law In Differential Form

Section 10.1 - Fields of Force

Section 10.2 - Voltage Related To Field

Section 10.3 - Fields by Superposition

Section 10.4 - Energy In Fields

Section 10.5 - LRC Circuits

Section 10.6 - Fields by Gauss' Law

Section 10.7 - Gauss' Law In Differential Form

“Okay. Your duties are as follows: Get Breen. I don't care how you get him, but get him soon. That faker! He posed for twenty years as a scientist without ever being apprehended. Well, I'm going to do some apprehending that'll make all previous apprehending look like no apprehension at all. You with me?”

“Yes,” said Battle, very much confused. “What's that thing you have?”

“Piggy-back heat-ray. You transpose the air in its path into an unstable isotope which tends to carry all energy as heat. Then you shoot your juice light, or whatever along the isotopic path and you burn whatever's on the receiving end. You want a few?”

“No,” said Battle. “I have my gats. What else have you got for offense and defense?” Underbottam opened a cabinet and proudly waved an arm. “Everything,” he said.

“Disintegraters, heat-rays, bombs of every type. And impenetrable shields of energy, massive and portable. What more do I need?”

From THE REVERSIBLE REVOLUTIONS by Cecil Corwin, Cosmic Stories, March 1941. Art by Morey, Bok, Kyle, Hunt, Forte. Copyright expired. }

Cutting-edge science readily infiltrates popular culture,
though sometimes in garbled form. The Newtonian imagination
populated the universe mostly with that nice solid stuff
called matter, which was made of little hard balls called
atoms. In the early twentieth century, consumers of pulp
fiction and popularized science began to hear of a new image
of the universe, full of x-rays, N-rays, and Hertzian waves.
What they were beginning to soak up through their skins was
a drastic revision of Newton's concept of a universe made of
chunks of matter which happened to interact via forces. In
the newly emerging picture, the universe was *made* of
force, or, to be more technically accurate, of ripples in
universal fields of force. Unlike the average reader of
Cosmic Stories in 1941, you now possess enough technical
background to understand what a “force field” really is.

What convinced physicists that they needed this new concept of a field of force? Although we have been dealing mostly with electrical forces, let's start with a magnetic example. (In fact the main reason I've delayed a detailed discussion of magnetism for so long is that mathematical calculations of magnetic effects are handled much more easily with the concept of a field of force.) First a little background leading up to our example. A bar magnet, a, has an axis about which many of the electrons' orbits are oriented. The earth itself is also a magnet, although not a bar-shaped one. The interaction between the earth-magnet and the bar magnet, b, makes them want to line up their axes in opposing directions (in other words such that their electrons rotate in parallel planes, but with one set rotating clockwise and the other counterclockwise as seen looking along the axes). On a smaller scale, any two bar magnets placed near each other will try to align themselves head-to-tail, c.

Now we get to the relevant example. It is clear that two people separated by a paper-thin wall could use a pair of bar magnets to signal to each other. Each person would feel her own magnet trying to twist around in response to any rotation performed by the other person's magnet. The practical range of communication would be very short for this setup, but a sensitive electrical apparatus could pick up magnetic signals from much farther away. In fact, this is not so different from what a radio does: the electrons racing up and down the transmitting antenna create forces on the electrons in the distant receiving antenna. (Both magnetic and electric forces are involved in real radio signals, but we don't need to worry about that yet.)

A question now naturally arises as to whether there is any time delay in this kind of communication via magnetic (and electric) forces. Newton would have thought not, since he conceived of physics in terms of instantaneous action at a distance. We now know, however, that there is such a time delay. If you make a long-distance phone call that is routed through a communications satellite, you should easily be able to detect a delay of about half a second over the signal's round trip of 50,000 miles. Modern measurements have shown that electric, magnetic, and gravitational forces all travel at the speed of light, \(3\times10^8\) m/s. (In fact, we will soon discuss how light itself is made of electricity and magnetism.)

If it takes some time for forces to be transmitted through
space, then apparently there is some *thing* that
travels *through* space. The fact that the phenomenon
travels outward at the same speed in all directions strongly
evokes wave metaphors such as ripples on a pond.

The smoking-gun argument for this strange notion of traveling force ripples comes from the fact that they carry energy.

First suppose that the person holding the bar magnet on the right decides to reverse hers, resulting in configuration d. She had to do mechanical work to twist it, and if she releases the magnet, energy will be released as it flips back to c. She has apparently stored energy by going from c to d. So far everything is easily explained without the concept of a field of force.

But now imagine that the two people start in position c
and then simultaneously flip their magnets extremely quickly
to position e, keeping them lined up with each other the
whole time. Imagine, for the sake of argument, that they can
do this so quickly that each magnet is reversed while the
force signal from the other is still in transit. (For a more
realistic example, we'd have to have two radio antennas, not
two magnets, but the magnets are easier to visualize.)
During the flipping, each magnet is still feeling the forces
arising from the way the other magnet *used* to be
oriented. Even though the two magnets stay aligned during
the flip, the time delay causes each person to feel
resistance as she twists her magnet around. How can this be?
Both of them are apparently doing mechanical work, so they
must be storing magnetic energy somehow. But in the
traditional Newtonian conception of matter interacting via
instantaneous forces at a distance, interaction energy arises
from the relative positions of objects that are interacting
via forces. If the magnets never changed their orientations
relative to each other, how can any magnetic energy have been stored?

The only possible answer is that the energy must have gone into the magnetic force ripples crisscrossing the space between the magnets. Fields of force apparently carry energy across space, which is strong evidence that they are real things.

This is perhaps not as radical an idea to us as it was to our ancestors. We are used to the idea that a radio transmitting antenna consumes a great deal of power, and somehow spews it out into the universe. A person working around such an antenna needs to be careful not to get too close to it, since all that energy can easily cook flesh (a painful phenomenon known as an “RF burn”).

Given that fields of force are real, how do we define, measure, and calculate them? A fruitful metaphor will be the wind patterns experienced by a sailing ship. Wherever the ship goes, it will feel a certain amount of force from the wind, and that force will be in a certain direction. The weather is ever-changing, of course, but for now let's just imagine steady wind patterns. Definitions in physics are operational, i.e., they describe how to measure the thing being defined. The ship's captain can measure the wind's “field of force” by going to the location of interest and determining both the direction of the wind and the strength with which it is blowing. Charting all these measurements on a map leads to a depiction of the field of wind force like the one shown in the figure. This is known as the “sea of arrows” method of visualizing a field.

Now let's see how these concepts are applied to the fundamental force fields of the universe. We'll start with the gravitational field, which is the easiest to understand. As with the wind patterns, we'll start by imagining gravity as a static field, even though the existence of the tides proves that there are continual changes in the gravity field in our region of space. When the gravitational field was introduced in chapter 2, I avoided discussing its direction explicitly, but defining it is easy enough: we simply go to the location of interest and measure the direction of the gravitational force on an object, such as a weight tied to the end of a string.

In chapter 2, I defined the gravitational field in
terms of the energy required to raise a unit mass through a unit distance.
However, I'm going to give a different definition now, using an
approach that will be more easily adapted to electric and magnetic fields.
This approach is based on force rather than energy.
We couldn't carry out the energy-based definition without dividing by
the mass of the object involved, and the same is true for the force-based definition.
For example, gravitational forces are weaker on the moon than on
the earth, but we cannot specify the strength of gravity
simply by giving a certain number of newtons. The number of
newtons of gravitational force depends not just on the
strength of the local gravitational field but also on the
mass of the object on which we're testing gravity, our
“test mass.” A boulder on the moon feels a stronger
gravitational force than a pebble on the earth. We can get
around this problem by defining the strength of the
gravitational field as the force acting on an object,
*divided by the object's mass:*

The gravitational field vector, \(\mathbf{g}\), at any location in space is found by placing a test mass \(m_t\) at that point. The field vector is then given by \(\mathbf{g}=\mathbf{F}/m_t\), where \(\mathbf{F}\) is the gravitational force on the test mass.

We now have three ways of representing a gravitational field. The magnitude of the gravitational field near the surface of the earth, for instance, could be written as 9.8 N/kg, 9.8 \(\text{J}/\text{kg}\cdot\text{m}\), or 9.8 \(\text{m}/\text{s}^2\). If we already had two names for it, why invent a third? The main reason is that it prepares us with the right approach for defining other fields.

The most subtle point about all this is that the gravitational
field tells us about what forces *would* be exerted on
a test mass by the earth, sun, moon, and the rest of the
universe, *if* we inserted a test mass at the point in
question. The field still exists at all the places where
we didn't measure it.

\(\triangleright\) Substituting \(|\mathbf{F}|= GMm_{t}/ r^2\) into the definition of the gravitational field, we find \(|\mathbf{g}|= GM/ r^2\). This expression could be used for the field of any spherically symmetric mass distribution, since the equation we assumed for the gravitational force would apply in any such case.

If we make a sea-of-arrows picture of the gravitational fields surrounding the earth, g, the result is evocative of water going down a drain. For this reason, anything that creates an inward-pointing field around itself is called a sink. The earth is a gravitational sink. The term “source” can refer specifically to things that make outward fields, or it can be used as a more general term for both “outies” and “innies.” However confusing the terminology, we know that gravitational fields are only attractive, so we will never find a region of space with an outward-pointing field pattern.

Knowledge of the field is interchangeable with knowledge of its sources (at least in the case of a static, unchanging field). If aliens saw the earth's gravitational field pattern they could immediately infer the existence of the planet, and conversely if they knew the mass of the earth they could predict its influence on the surrounding gravitational field.

A very important fact about all fields of force is that when there is more than one source (or sink), the fields add according to the rules of vector addition. The gravitational field certainly will have this property, since it is defined in terms of the force on a test mass, and forces add like vectors. Superposition is an important characteristics of waves, so the superposition property of fields is consistent with the idea that disturbances can propagate outward as waves in a field.

\(\triangleright\) The average gravitational field on Jupiter's moon Io is 1.81 N/kg. By how much is this reduced when Jupiter is directly overhead? Io's orbit has a radius of \( 4.22\times10^8\) m, and Jupiter's mass is \( 1.899\times10^{27}\) kg.

\(\triangleright\) By the shell theorem, we can treat the Jupiter as if its mass was all concentrated at its center, and likewise for Io. If we visit Io and land at the point where Jupiter is overhead, we are on the same line as these two centers, so the whole problem can be treated one-dimensionally, and vector addition is just like scalar addition. Let's use positive numbers for downward fields (toward the center of Io) and negative for upward ones. Plugging the appropriate data into the expression derived in example 1, we find that the Jupiter's contribution to the field is \(- 0.71\) N/kg. Superposition says that we can find the actual gravitational field by adding up the fields created by Io and Jupiter: \(1.81-0.71\) N/kg = 1.1 N/kg. You might think that this reduction would create some spectacular effects, and make Io an exciting tourist destination. Actually you would not detect any difference if you flew from one side of Io to the other. This is because your body and Io both experience Jupiter's gravity, so you follow the same orbital curve through the space around Jupiter.

A source that sits still will create a static field pattern, like a steel ball sitting peacefully on a sheet of rubber. A moving source will create a spreading wave pattern in the field, like a bug thrashing on the surface of a pond. Although we have started with the gravitational field as the simplest example of a static field, stars and planets do more stately gliding than thrashing, so gravitational waves are not easy to detect. Newton's theory of gravity does not describe gravitational waves, but they are predicted by Einstein's general theory of relativity. J.H. Taylor and R.A. Hulse were awarded the Nobel Prize in 1993 for giving indirect evidence that Einstein's waves actually exist. They discovered a pair of exotic, ultra-dense stars called neutron stars orbiting one another very closely, and showed that they were losing orbital energy at the rate predicted by Einstein's theory.

A Caltech-MIT collaboration has built a pair of gravitational wave detectors called LIGO to search for more direct evidence of gravitational waves. Since they are essentially the most sensitive vibration detectors ever made, they are located in quiet rural areas, and signals will be compared between them to make sure that they were not due to passing trucks. The project began operating at full sensitivity in 2005, and is now able to detect a vibration that causes a change of \(10^{-18}\) m in the distance between the mirrors at the ends of the 4-km vacuum tunnels. This is a thousand times less than the size of an atomic nucleus! There is only enough funding to keep the detectors operating for a few more years, so the physicists can only hope that during that time, somewhere in the universe, a sufficiently violent cataclysm will occur to make a detectable gravitational wave. (More accurately, they want the wave to arrive in our solar system during that time, although it will have been produced millions of years before.)

The definition of the electric field is directly analogous to, and has the same motivation as, the definition of the gravitational field:

The electric field vector, \(\mathbf{E}\), at any location in space is found by placing a test charge \(q_t\) at that point. The electric field vector is then given by \(\mathbf{E}=\mathbf{F}/q_t\), where \(\mathbf{F}\) is the electric force on the test charge.

Charges are what create electric fields. Unlike gravity, which is always attractive, electricity displays both attraction and repulsion. A positive charge is a source of electric fields, and a negative one is a sink.

The most difficult point about the definition of the electric field is that the force on a negative charge is in the opposite direction compared to the field. This follows from the definition, since dividing a vector by a negative number reverses its direction. It's as though we had some objects that fell upward instead of down.

Find an equation for the magnitude of the field of a single point charge \(Q\).

(answer in the back of the PDF version of the book)\(\triangleright\) The field at P is the vector sum of the fields that would have been created by the two charges independently. Let positive \(x\) be to the right and let positive \(y\) be up.

Negative charges have fields that point at them, so the charge \(-q\) makes a field that points to the right, i.e., has a positive \(x\) component. Using the answer to the self-check, we have

\[\begin{align*}
E_{-q,x} &= \frac{ kq}{ b^2} \\
E_{-q,y} &= 0 .
\end{align*}\]

Note that if we had blindly ignored the absolute value signs and plugged in \(- q\) to the equation, we would have incorrectly concluded that the field went to the left.

By the Pythagorean theorem, the positive charge is at a
distance \(\sqrt{2} b\) from P, so the magnitude of its contribution to
the field is \(E= kq/2 b^2\). Positive charges have
fields that point away from them, so the field vector is at
an angle of 135° counterclockwise from the \(x\) axis.

\[\begin{align*}
E_{q,x} &= \frac{ kq}{2 b^2} \text{cos}\ 135° \\
&= -\frac{ kq}{2^\text{3/2} b^2} \\
E_{q,y} &= \frac{ kq}{2 b^2} \text{sin}\ 135° \\
&= \frac{ kq}{2^\text{3/2} b^2}
\end{align*}\]

The total field is

\[\begin{align*}
E_\text{x} &= \left(1-2^{-\text{3/2}}\right)\frac{ kq}{ b^2} \\
E_{y} &= \frac{ kq}{2^\text{3/2} b^2}
\end{align*}\]

The simplest set of sources that can occur with electricity
but not with gravity is the *dipole*,
consisting of a positive charge and a negative charge
with equal magnitudes. More generally, an electric dipole can
be any object with an imbalance of positive charge on one
side and negative on the other. A water molecule, l, is a
dipole because the electrons tend to shift away from the
hydrogen atoms and onto the oxygen atom.

Your microwave oven acts on water molecules with electric fields. Let us imagine what happens if we start with a uniform electric field, m/1, made by some external charges, and then insert a dipole, m/2, consisting of two charges connected by a rigid rod. The dipole disturbs the field pattern, but more important for our present purposes is that it experiences a torque. In this example, the positive charge feels an upward force, but the negative charge is pulled down. The result is that the dipole wants to align itself with the field, m/3. The microwave oven heats food with electrical (and magnetic) waves. The alternation of the torque causes the molecules to wiggle and increase the amount of random motion. The slightly vague definition of a dipole given above can be improved by saying that a dipole is any object that experiences a torque in an electric field.

What determines the torque on a dipole placed in an externally created field? Torque depends on the force, the distance from the axis at which the force is applied, and the angle between the force and the line from the axis to the point of application. Let a dipole consisting of charges \(+q\) and \(-q\) separated by a distance \(\ell\) be placed in an external field of magnitude \(|\mathbf{E}|\), at an angle \(\theta\) with respect to the field. The total torque on the dipole is

\[\begin{align*}
\tau &= \frac{\ell}{2}q|\mathbf{E}|\sin \theta+\frac{\ell}{2}q|\mathbf{E}|\sin \theta \\
&= \ell q|\mathbf{E}|\sin \theta .
\end{align*}\]

(Note that even though the two forces are in opposite directions, the torques do not cancel, because they are both trying to twist the dipole in the same direction.) The quantity is called the dipole moment, notated \(D\). (More complex dipoles can also be assigned a dipole moment --- they are defined as having the same dipole moment as the two-charge dipole that would experience the same torque.)

Employing a little more mathematical elegance, we can define
a dipole moment *vector*,

\[\begin{equation*}
\mathbf{D} = \sum q_i \mathbf{r}_i ,
\end{equation*}\]

where \(\mathbf{r}_i\) is the position vector of the charge labeled by the index \(i\). We can then write the torque in terms of a vector cross product (page 281),

\[\begin{equation*}
\boldsymbol{\tau} = \mathbf{D}\times\mathbf{E} .
\end{equation*}\]

No matter how we notate it, the definition of the dipole moment requires that we choose point from which we measure all the position vectors of the charges. However, in the commonly encountered special case where the total charge of the object is zero, the dipole moment is the same regardless of this choice.

\(\triangleright\) In a molecule of NaCl gas, the center-to-center distance between the two atoms is about 0.6 nm. Assuming that the chlorine completely steals one of the sodium's electrons, compute the magnitude of this molecule's dipole moment.

\(\triangleright\) The total charge is zero, so it doesn't matter where we choose the origin of our coordinate system. For convenience, let's choose it to be at one of the atoms, so that the charge on that atom doesn't contribute to the dipole moment. The magnitude of the dipole moment is then

\[\begin{align*}
D &= (6\times10^{-10}\ \text{m})( e) \\
&= (6\times10^{-10}\ \text{m})( 1.6\times10^{-19}\ \text{C}) \\
&= 1\times10^{-28}\ \text{C}\cdot\text{m}
\end{align*}\]

\(\triangleright\) Let the origin of the coordinate system be at the leftmost charge.

\[\begin{align*}
\mathbf{D} &= \sum q_i \mathbf{r}_i \\
&= (q)(\vc{0})+(-q)(b\hat{\mathbf{x}})+(q)(b\hat{\mathbf{x}}+b\hat{\mathbf{y}})+(-q)(2b\hat{\mathbf{x}}) \\
&= -2bq\hat{\mathbf{x}}+bq\hat{\mathbf{y}}
\end{align*}\]

The behavior of a dipole in an externally created field leads us to an alternative definition of the electric field:

The electric field vector, \(E\), at any location in space is defined by observing the torque exerted on a test dipole \(D_t\) placed there. The direction of the field is the direction in which the field tends to align a dipole (from \(-\) to +), and the field's magnitude is \(|\mathbf{E}|=\tau/D_t\sin\theta\). In other words, the field vector is the vector that satisfies the equation \(\boldsymbol{\tau} = \mathbf{D}_t\times\mathbf{E}\) for any test dipole \(\mathbf{D}_t\) placed at that point in space.

The main reason for introducing a second definition for the same concept is that the magnetic field is most easily defined using a similar approach.

◊

In the definition of the electric field, does the test charge need to be 1 coulomb? Does it need to be positive?

◊

Does a charged particle such as an electron or proton feel a force from its own electric field?

◊

Is there an electric field surrounding a wall socket that has nothing plugged into it, or a battery that is just sitting on a table?

◊

In a flashlight powered by a battery, which way do the electric fields point? What would the fields be like inside the wires? Inside the filament of the bulb?

◊

Criticize the following statement: “An electric field can be represented by a sea of arrows showing how current is flowing.”

◊

The field of a point charge, \(|\mathbf{E}|=kQ/r^2\), was derived in a self-check. How would the field pattern of a uniformly charged sphere compare with the field of a point charge?

◊

The interior of a perfect electrical conductor in equilibrium must have zero electric field, since otherwise the free charges within it would be drifting in response to the field, and it would not be in equilibrium. What about the field right at the surface of a perfect conductor? Consider the possibility of a field perpendicular to the surface or parallel to it.

◊

Small pieces of paper that have not been electrically prepared in any way can be picked up with a charged object such as a charged piece of tape. In our new terminology, we could describe the tape's charge as inducing a dipole moment in the paper. Can a similar technique be used to induce not just a dipole moment but a charge?

Voltage is electrical energy per unit charge, and electric field is force per unit charge. For a particle moving in one dimension, along the \(x\) axis, we can therefore relate voltage and field if we start from the relationship between interaction energy and force,

\[\begin{equation*}
dU = -F_xdx ,
\end{equation*}\]

and divide by charge,

\[\begin{equation*}
\frac{dU}{q} = -\frac{F_x}{q}dx ,
\end{equation*}\]

giving

\[\begin{equation*}
dV = -E_x dx ,
\end{equation*}\]

or

\[\begin{equation*}
\frac{dV}{dx} = -E_x .
\end{equation*}\]

The interpretation is that a strong electric field occurs in a region of space where the voltage is rapidly changing. By analogy, a steep hillside is a place on the map where the altitude is rapidly changing.

\(\triangleright\) Suppose an electric eel is 1 m long, and generates a voltage difference of 1000 volts between its head and tail. What is the electric field in the water around it?

\(\triangleright\) We are only calculating the amount of field, not its direction, so we ignore positive and negative signs. Subject to the possibly inaccurate assumption of a constant field parallel to the eel's body, we have

\[\begin{align*}
|\mathbf{E}| &= \frac{dV}{d x} \\
&\approx \frac{\Delta V}{\Delta x} \text{[assumption of constant field]} \\
&= 1000\ \text{V/m} .
\end{align*}\]

From our original definition of the electric field, we expect it to have units of newtons per coulomb, N/C. The example above, however, came out in volts per meter, V/m. Are these inconsistent? Let's reassure ourselves that this all works. In this kind of situation, the best strategy is usually to simplify the more complex units so that they involve only mks units and coulombs. Since voltage is defined as electrical energy per unit charge, it has units of J/C:

\[\begin{align*}
\frac{\text{V}}{\text{m}} &= \frac{\text{J/C}}{\text{m}} \\
&= \frac{\text{J}}{\text{C}\cdot\text{m}} .
\end{align*}\]

To connect joules to newtons, we recall that work equals force times distance, so \(\text{J}=\text{N}\cdot\text{m}\), so

\[\begin{align*}
\frac{\text{V}}{\text{m}} &= \frac{\text{N}\cdot\text{m}}{\text{C}\cdot\text{m}} \\
&= \frac{\text{N}}{\text{C}}
\end{align*}\]

As with other such difficulties with electrical units, one quickly begins to recognize frequently occurring combinations.

\(\triangleright\) What is the voltage associated with a point charge?

\(\triangleright\) As derived previously in self-check A on page 565, the field is

\[\begin{equation*}
|\mathbf{E}| = \frac{ kQ}{ r^2}
\end{equation*}\]

The difference in voltage between two points on the same radius line is

\[\begin{align*}
\Delta V &= -\int d V \\
&= -\int E_{x} d x
\end{align*}\]

In the general discussion above, \(x\) was just a generic name for distance traveled along the line from one point to the other, so in this case \(x\) really means \(r\).

\[\begin{align*}
\Delta V &= -\int_{ r_1}^{ r_2} E_{r} d r \\
&= -\int_{ r_1}^{ r_2} \frac{ kQ}{ r^2} d r \\
&= \left.\frac{ kQ}{ r}\right]_{ r_1}^{ r_2} \
&= \frac{ kQ}{ r_2}-\frac{ kQ}{ r_1} .
\end{align*}\]

The standard convention is to use \(r_1=\infty\) as a reference point, so that the voltage at any distance \(r\) from the charge is

\[\begin{equation*}
V = \frac{ kQ}{ r} .
\end{equation*}\]

The interpretation is that if you bring a positive test charge closer to a positive charge, its electrical energy is increased; if it was released, it would spring away, releasing this as kinetic energy.

Show that you can recover the expression for the field of a point charge by evaluating the derivative \(E_{x}=-d V/d x\).

(answer in the back of the PDF version of the book)The topographical map in figure a suggests a good way to visualize the relationship between field and voltage in two dimensions. Each contour on the map is a line of constant height; some of these are labeled with their elevations in units of feet. Height is related to gravitational energy, so in a gravitational analogy, we can think of height as representing voltage. Where the contour lines are far apart, as in the town, the slope is gentle. Lines close together indicate a steep slope.

If we walk along a straight line, say straight east from the town, then height (voltage) is a function of the east-west coordinate \(x\). Using the usual mathematical definition of the slope, and writing \(V\) for the height in order to remind us of the electrical analogy, the slope along such a line is \(dV/dx\) (the rise over the run).

What if everything isn't confined to a straight line? Water flows downhill. Notice how the streams on the map cut perpendicularly through the lines of constant height.

It is possible to map voltages in the same way, as shown in figure b. The electric field is strongest where the constant-voltage curves are closest together, and the electric field vectors always point perpendicular to the constant-voltage curves.

The one-dimensional relationship \(E=-dV/dx\) generalizes to three dimensions as follows:

\[\begin{align*}
E_x &= -\frac{dV}{dx} \\
E_y &= -\frac{dV}{dy} \\
E_z &= -\frac{dV}{dz}
\end{align*}\]

This can be notated as a gradient (page 215),

\[\begin{equation*}
\mathbf{E} = \nabla V ,
\end{equation*}\]

and if we know the field and want to find the voltage, we can use a line integral,

\[\begin{equation*}
\Delta V = \int_C \mathbf{E}\cdotd\mathbf{r} ,
\end{equation*}\]

where the quantity inside the integral is a vector dot product.

Imagine that figure a represents voltage rather than height. (a) Consider the stream the starts near the center of the map. Determine the positive and negative signs of \(dV/dx\) and \(dV/dy\), and relate these to the direction of the force that is pushing the current forward against the resistance of friction. (b) If you wanted to find a lot of electric charge on this map, where would you look?

(answer in the back of the PDF version of the book)Figure c shows some examples of ways to visualize field and voltage patterns.

Charge really comes in discrete chunks, but often it is mathematically convenient to treat a set of charges as if they were like a continuous fluid spread throughout a region of space. For example, a charged metal ball will have charge spread nearly uniformly all over its surface, and for most purposes it will make sense to ignore the fact that this uniformity is broken at the atomic level. The electric field made by such a continuous charge distribution is the sum of the fields created by every part of it. If we let the “parts” become infinitesimally small, we have a sum of an infinitely many infinitesimal numbers: an integral. If it was a discrete sum, as in example 3 on page 566, we would have a total electric field in the \(x\) direction that was the sum of all the \(x\) components of the individual fields, and similarly we'd have sums for the \(y\) and \(z\) components. In the continuous case, we have three integrals. Let's keep it simple by starting with a one-dimensional example.

\(\triangleright\) This is a one-dimensional situation, so we really only need to do a single integral representing the total field along the axis. We imagine breaking the rod down into short pieces of length \(d z\), each with charge \(d q\). Since charge is uniformly spread along the rod, we have \(d q=\lambdad z\), where \(\lambda= Q/ L\) (Greek lambda) is the charge per unit length, in units of coulombs per meter. Since the pieces are infinitesimally short, we can treat them as point charges and use the expression \(kd q/ r^2\) for their contributions to the field, where \(r= d- z\) is the distance from the charge at \(z\) to the point in which we are interested.

\[\begin{align*}
E_{z} &= \int \frac{ kd q }{ r^2} \\
&= \int_{- L/2}^{+ L/2} \frac{ k\lambdad z }{ r^2} \\
&= k \lambda \int_{- L/2}^{+ L/2} \frac{d z}{( d- z)^2}
\end{align*}\]

The integral can be looked up in a table, or reduced to an elementary form by substituting a new variable for \(d- z\). The result is

\[\begin{align*}
E_{z} &= k\lambda\left(\frac{1}{ d- z}\right)_{- L/2}^{+ L/2} \\
&= \frac{ kQ}{ L} \left(\frac{1}{ d- L/2}-\frac{1}{ d+ L/2}\right) .
\end{align*}\]

For large values of \(d\), this expression gets smaller for two reasons: (1) the denominators of the fractions become large, and (2) the two fractions become nearly the same, and tend to cancel out. This makes sense, since the field should get weaker as we get farther away from the charge. In fact, the field at large distances must approach \( kQ/ d^2\) (homework problem 2).

It's also interesting to note that the field becomes infinite at the ends of the rod, but is not infinite on the interior of the rod. Can you explain physically why this happens?

Example 9 was one-dimensional. In the general three-dimensional case, we might have to integrate all three components of the field. However, there is a trick that lets us avoid this much complication. The voltage is a scalar, so we can find the voltage by doing just a single integral, then use the voltage to find the field.

\(\triangleright\) By symmetry, the field has only a radial component, \(E_R\), pointing directly away from the rod (or toward it for \(Q\lt0\)). The brute-force approach, then, would be to evaluate the integral \(E=\int |d\mathbf{E}|\text{cos}\ \theta\), where \(d\mathbf{E}\) is the contribution to the field from a charge \(dq\) at some point along the rod, and \(\theta\) is the angle \(d\mathbf{E}\) makes with the radial line.

It's easier, however, to find the voltage first, and then find the field from the voltage. Since the voltage is a scalar, we simply integrate the contribution \(dV\) from each charge \(dq\), without even worrying about angles and directions. Let \(z\) be the coordinate that measures distance up and down along the rod, with \(z=0\) at the center of the rod. Then the distance between a point \(z\) on the rod and the point of interest is \(r=\sqrt{ z^2+ R^2}\), and we have

\[\begin{align*}
V &= \int \frac{ kdq}{ r} \\
&= k\lambda \int_{- L/2}^{+ L/2}\frac{dz}{ r} \\
&= k\lambda \int_{- L/2}^{+ L/2}\frac{dz}{\sqrt{ z^2+ R^2}} \\
\end{align*}\]

The integral can be looked up in a table, or evaluated using computer software:

\[\begin{align*}
V &= \left. k\lambda\: \text{ln}\left( z+\sqrt{ z^2+ R^2}\right)\right|_{- L/2}^{+ L/2} \\
&= k\lambda\: \text{ln}\left(\frac{ L/2+\sqrt{ L^2/4+ R^2}}{- L/2+\sqrt{ L^2/4+ R^2}}\right) \\
\end{align*}\]

The expression inside the parentheses can be simplified a little. Leaving out some tedious algebra, the result is

\[\begin{equation*}
V = 2 k\lambda\: \text{ln}\left(\frac{ L}{2 R}+\sqrt{1+\frac{ L^2}{4 R^2}}\right)
\end{equation*}\]

This can readily be differentiated to find the field:

\[\begin{align*}
E_{R} &= -\frac{dV}{dR} \\
&= (-2 k\lambda)\frac{- L/2 R^2
+(1/2)(1+ L^2/4 R^2)^{-1/2}(- L^2/2 R^3)
}{L/2 R+(1+ L^2/4 R^2)^{1/2}
} , \\
\text{or, after some simplification,}
E_{R} &= \frac{ k\lambda L}{ R^2\sqrt{1+ L^2/4 R^2}}
\end{align*}\]

For large values of \(R\), the square root approaches one, and we have simply \(E_{R}\approx k\lambda L/ R^2= k Q/ R^2\). In other words, the field very far away is the same regardless of whether the charge is a point charge or some other shape like a rod. This is intuitively appealing, and doing this kind of check also helps to reassure one that the final result is correct.

The preceding example, although it involved some messy algebra, required only straightforward calculus, and no vector operations at all, because we only had to integrate a scalar function to find the voltage. The next example is one in which we can integrate either the field or the voltage without too much complication.

\(\triangleright\) Integrating the voltage is straightforward.

\[\begin{align*}
V &= \int \frac{ kdq}{ r} \\
&= k \int \frac{dq}{\sqrt{ b^2+ z^2}} \\
&= \frac{ k}{\sqrt{ b^2+ z^2}} \int dq \\
&= \frac{ kQ}{\sqrt{ b^2+ z^2}} ,
\end{align*}\]

where \(Q\) is the total charge of the ring. This result could have been derived without calculus, since the distance \(r\) is the same for every point around the ring, i.e., the integrand is a constant. It would also be straightforward to find the field by differentiating this expression with respect to \(z\) (homework problem 10).

Instead, let's see how to find the field by direct integration. By symmetry, the field at the point of interest can have only a component along the axis of symmetry, the \(z\) axis:

\[\begin{align*}
E_{x} &= 0 \\
E_y &= 0
\end{align*}\]

To find the field in the \(z\) direction, we integrate the \(z\) components contributed to the field by each infinitesimal part of the ring.

\[\begin{align*}
E_{z} &= \int dE_z \\
&= \int |d\mathbf{E}|\:\text{cos}\:\theta ,
\end{align*}\]

where \(\theta\) is the angle shown in the figure.

\[\begin{align*}
E_{z} &= \int \frac{ kdq}{ r^2}\:\text{cos}\:\theta \\
&= k \int \frac{dq}{ b^2+ z^2}\:\text{cos}\:\theta
\end{align*}\]

Everything inside the integral is a constant, so we have

\[\begin{align*}
E_{z} &= \frac{ k}{ b^2+ z^2}\:\text{cos}\:\theta \int dq \\
&= \frac{ kQ}{ b^2+ z^2}\:\text{cos}\:\theta \\
&= \frac{ kQ}{ b^2+ z^2}\:\frac{ z}{ r} \\
&= \frac{ kQz}{\left( b^2+ z^2\right)^\text{3/2}}
\end{align*}\]

In all the examples presented so far, the charge has been confined to a one-dimensional line or curve. Although it is possible, for example, to put charge on a piece of wire, it is more common to encounter practical devices in which the charge is distributed over a two-dimensional surface, as in the flat metal plates used in Thomson's experiments. Mathematically, we can approach this type of calculation with the divide-and-conquer technique: slice the surface into lines or curves whose fields we know how to calculate, and then add up the contributions to the field from all these slices. In the limit where the slices are imagined to be infinitesimally thin, we have an integral.

\(\triangleright\) We're given that every part of the disk has the same charge per unit area, so rather than working with \(Q\), the total charge, it will be easier to use the charge per unit area, conventionally notated \(\sigma\) (Greek sigma), \(\sigma= Q/\pi b^2\).

Since we already know the field due to a ring of charge, we can solve the problem by slicing the disk into rings, with each ring extending from \(r\) to \(r+dr\). The area of such a ring equals its circumference multiplied by its width, i.e., \(2\pi rdr\), so its charge is \(dq=2\pi\sigma rdr\), and from the result of example 11, its contribution to the field is

\[\begin{align*}
dE_{z} &= \frac{ kzdq}{\left( r^2+ z^2\right)^\text{3/2}} \\
&= \frac{2\pi\sigma kzrdr}{\left( r^2+ z^2\right)^\text{3/2}} \\
\end{align*}\]

The total field is

\[\begin{align*}
E_{z} &= \int dE_{z} \\
&= 2\pi\sigma kz
\int_0^{b}
\frac{ rdr}{\left( r^2+ z^2\right)^\text{3/2}} \\
&= 2\pi\sigma kz \left. \frac{-1}{\sqrt{ r^2+ z^2}}
\right|_{ r=0}^{ r=\text{b}} \\
&= 2\pi\sigma k\left(1-\frac{ z}{\sqrt{ b^2+ z^2}}\right)
\end{align*}\]

The result of example 12 has some interesting properties. First, we note that it was derived on the unspoken assumption of \(z>0\). By symmetry, the field on the other side of the disk must be equally strong, but in the opposite direction, as shown in figures e and g. Thus there is a discontinuity in the field at \(z=0\). In reality, the disk will have some finite thickness, and the switching over of the field will be rapid, but not discontinuous.

At large values of \(z\), i.e., \(z\gg b\), the field rapidly approaches the \(1/r^2\) variation that we expect when we are so far from the disk that the disk's size and shape cannot matter (homework problem 2).

A practical application is the case of a capacitor, f, having
two parallel circular plates very close together. In normal operation, the charges
on the plates are opposite, so one plate has fields pointing into it and the other
one has fields pointing out. In a real capacitor, the plates are a metal conductor,
not an insulator, so the charge will tend to arrange itself more densely near the edges,
rather than spreading itself uniformly on each plate. Furthermore, we have only calculated
the *on-axis* field in example 12; in the off-axis region,
each disk's contribution
to the field will be weaker, and it will also point away from the axis a little. But if we are
willing to ignore these complications for the sake of a rough analysis, then the fields
superimpose as shown in figure f: the fields cancel the outside of the
capacitor, but between the plates its value is double that contributed by a single
plate. This cancellation on the outside is a very useful property for a practical
capacitor. For instance, if you look at the printed circuit board in a typical piece
of consumer electronics, there are many capacitors, often placed fairly close together.
If their exterior fields didn't cancel out nicely, then each capacitor would interact
with its neighbors in a complicated way, and the behavior of the circuit would depend
on the exact physical layout, since the interaction would be stronger or weaker depending
on distance. In reality, a capacitor does create weak external electric fields, but their
effects are often negligible, and we can then use the *lumped-circuit approximation*,
which states that each component's behavior depends only on the currents that flow in
and out of it, not on the interaction of its fields with the other components.

From a theoretical point of view, there is something even more intriguing about example 12: the magnitude of the field for small values of \(z\) (\(z\ll b\)) is \(E=2\pi k\sigma\), which doesn't depend on \(b\) at all for a fixed value of \(\sigma\). If we made a disk with twice the radius, and covered it with the same number of coulombs per square meter (resulting in a total charge four times as great), the field close to the disk would be unchanged! That is, a flea living near the center of the disk, h, would have no way of determining the size of her flat “planet” by measuring the local field and charge density. (Only by leaping off the surface into outer space would she be able to measure fields that were dependent on \(b\). If she traveled very far, to \(z\gg b\), she would be in the region where the field is well approximated by \(|\mathbf{E}|\approx kQ/z^2=k\pi b^2\sigma/z^2\), which she could solve for \(b\).)

What is the reason for this surprisingly simple behavior of the field? Is it a
piece of mathematical trivia, true only in this particular case? What if the shape
was a square rather than a circle? In other words, the flea gets no information about
the *size* of the disk from measuring \(E\), since \(E=2\pi k\sigma\), independent
of \(b\), but what if she didn't know the *shape*, either? If the result for a square
had some other geometrical factor in front instead of \(2\pi\), then she could tell which
shape it was by measuring \(E\). The surprising mathematical fact, however, is that the
result for a square, indeed for any shape whatsoever, is \(E=2\pi\sigma k\). It doesn't
even matter whether the surface is flat or warped, or whether the density of charge
is different at parts of the surface which are far away compared to the flea's distance
above the surface.

This universal \(E_\perp=2\pi k\sigma\) field perpendicular to
a charged surface can be proved mathematically based
on Gauss's law^{1} (section 10.6), but we can understand
what's happening on qualitative grounds. Suppose on night, while the flea is asleep,
someone adds more surface area, also positively charged, around the outside edge of
her disk-shaped world, doubling its radius. The added charge, however, has very little
effect on the field in her environment, as long as she stays at low altitudes above
the surface. As shown in figure i, the new charge
to her west contributes a field, T, that is almost purely “horizontal” (i.e., parallel
to the surface) and to the east. It has
a negligible upward component, since the angle is so shallow. This new eastward
contribution to the field
is exactly canceled out by the westward field, S, created by the new charge to her east.
There is likewise almost perfect cancellation between any other pair of opposite
compass directions.

A similar argument can be made as to the shape-independence of the result, as long as the shape is symmetric. For example, suppose that the next night, the tricky real estate developers decide to add corners to the disk and transform it into a square. Each corner's contribution to the field measured at the center is canceled by the field due to the corner diagonally across from it.

What if the flea goes on a trip away from the center of the disk? The perfect cancellation of the “horizontal” fields contributed by distant charges will no longer occur, but the “vertical” field (i.e., the field perpendicular to the surface) will still be \(E_\perp=2\pi k\sigma\), where \(\sigma\) is the local charge density, since the distant charges can't contribute to the vertical field. The same result applies if the shape of the surface is asymmetric, and doesn't even have any well-defined geometric center: the component perpendicular to the surface is \(E_\perp=2\pi k\sigma\), but we may have \(E_\parallel\neq0\). All of the above arguments can be made more rigorous by discussing mathematical limits rather than using words like “very small.” There is not much point in giving a rigorous proof here, however, since we will be able to demonstrate this fact as a corollary of Gauss' Law in section 10.6. The result is as follows:

At a point lying a distance \(z\) from a charged surface, the component of the electric field perpendicular to the surface obeys

\[\begin{equation*}
\lim_{z\rightarrow 0} E_\perp = 2\pi k\sigma ,
\end{equation*}\]

where \(\sigma\) is the charge per unit area. This is true regardless of the shape or size of the surface.

\(\triangleright\) For a point charge, we have already found \(E\propto d^{-2}\) for the magnitude of the field, where we are now using \(d\) for the quantity we would ordinarily notate as \(r\). This is true for all values of \(d\), not just for small \(d\) --- it has to be that way, because the point charge has no size, so if \(E\) behaved differently for small and large \(d\), there would be no way to decide what \(d\) had to be small or large relative to.

For a line of charge, the result of example 10 is

\[\begin{equation*}
E = \frac{ k\lambda L}{ d^2\sqrt{1+ L^2/4 d^2}} .
\end{equation*}\]

In the limit of \(d\ll L\), the quantity inside the square root is dominated by the second term, and we have \(E\propto d^{-1}\).

Finally, in the case of a charged surface, the result is simply \(E=2\pi\sigma k\), or \(E\propto d^{0}\).

Notice the lovely simplicity of the pattern, as shown in figure j. A point is zero-dimensional: it has no length, width, or breadth. A line is one-dimensional, and a surface is two-dimensional. As the dimensionality of the charged object changes from 0 to 1, and then to 2, the exponent in the near-field expression goes from 2 to 1 to 0.

Fields possess energy, as argued on page 561, but how much energy?
The answer can be found using the following elegant approach. We assume that the electric energy
contained in an infinitesimal volume of space \(dv\) is given by
\(dU_e=f(\mathbf{E})dv\), where \(f\) is some function, which we wish to determine,
of the field **E**.
It might seem that we would have no easy way to determine the function \(f\), but many of
the functions we could cook up would violate the symmetry of space. For instance,
we could imagine \(f(\mathbf{E})=aE_y\), where \(a\) is some constant with the appropriate units.
However, this would violate the symmetry of space, because it would give the \(y\) axis
a different status from \(x\) and \(z\). As discussed on page 212,
if we wish to calculate a scalar based on some vectors, the dot product is the only way
to do it that has the correct symmetry properties. If all we have is one vector, **E**, then
the only scalar we can form is \(\mathbf{E}\cdot\mathbf{E}\), which is the square of the magnitude
of the electric field vector.

In principle, the energy function we are seeking could be proportional to \(\mathbf{E}\cdot\mathbf{E}\), or to any function computed from it, such as \(\sqrt{\mathbf{E}\cdot\mathbf{E}}\) or \((\mathbf{E}\cdot\mathbf{E})^7\). On physical grounds, however, the only possibility that works is \(\mathbf{E}\cdot\mathbf{E}\). Suppose, for instance, that we pull apart two oppositely charged capacitor plates, as shown in figure a. We are doing work by pulling them apart against the force of their electrical attraction, and this quantity of mechanical work equals the increase in electrical energy, \(U_e\). Using our previous approach to energy, we would have thought of \(U_e\) as a quantity which depended on the distance of the positive and negative charges from each other, but now we're going to imagine \(U_e\) as being stored within the electric field that exists in the space between and around the charges. When the plates are touching, their fields cancel everywhere, and there is zero electrical energy. When they are separated, there is still approximately zero field on the outside, but the field between the plates is nonzero, and holds some energy. Now suppose we carry out the whole process, but with the plates carrying double their previous charges. Since Coulomb's law involves the product \(q_1q_2\) of two charges, we have quadrupled the force between any given pair of charged particles, and the total attractive force is therefore also four times greater than before. This means that the work done in separating the plates is four times greater, and so is the energy \(U_e\) stored in the field. The field, however, has merely been doubled at any given location: the electric field \(\mathbf{E}_+\) due to the positively charged plate is doubled, and similarly for the contribution \(\mathbf{E}_-\) from the negative one, so the total electric field \(\mathbf{E}_++\mathbf{E}_-\) is also doubled. Thus doubling the field results in an electrical energy which is four times greater, i.e., the energy density must be proportional to the square of the field, \(dU_e\propto(\mathbf{E}\cdot\mathbf{E})dv\). For ease of notation, we write this as \(dU_e\propto E^2dv\), or \(dU_e=aE^2dv\), where \(a\) is a constant of proportionality. Note that we never really made use of any of the details of the geometry of figure a, so the reasoning is of general validity. In other words, not only is \(dU_e=aE^2dv\) the function that works in this particular case, but there is every reason to believe that it would work in other cases as well.

It now remains only to find \(a\). Since the constant must be the same in all situations, we only need to find one example in which we can compute the field and the energy, and then we can determine \(a\). The situation shown in figure a is just about the easiest example to analyze. We let the square capacitor plates be uniformly covered with charge densities \(+\sigma\) and \(-\sigma\), and we write \(b\) for the lengths of their sides. Let \(h\) be the gap between the plates after they have been separated. We choose \(h\ll b\), so that the field experienced by the negative plate due to the positive plate is \(E_+=2\pi k\sigma\). The charge of the negative plate is \(-\sigma b^2\), so the magnitude of the force attracting it back toward the positive plate is \((\text{force})=(\text{charge})(\text{field})=2\pi k\sigma^2 b^2\). The amount of work done in separating the plates is \((\text{work})=(\text{force})(\text{distance})=2\pi k\sigma^2 b^2h\). This is the amount of energy that has been stored in the field between the two plates, \(U_e=2\pi k\sigma^2 b^2h=2\pi k\sigma^2 v\), where \(v\) is the volume of the region between the plates.

We want to equate this to \(U_e=aE^2v\). (We can write \(U_e\) and \(v\) rather than \(dU_e\) and \(dv\), since the field is constant in the region between the plates.) The field between the plates has contributions from both plates, \(E=E_++E_-=4\pi k\sigma\). (We only used half this value in the computation of the work done on the moving plate, since the moving plate can't make a force on itself. Mathematically, each plate is in a region where its own field is reversing directions, so we can think of its own contribution to the field as being zero within itself.) We then have \(aE^2v=a\cdot 16\pi^2k^2\sigma^2 \cdot v\), and setting this equal to \(U_e=2\pi k\sigma^2 v\) from the result of the work computation, we find \(a=1/8\pi k\). Our final result is as follows:

The electric energy possessed by an electric field **E** occupying an infinitesimal
volume of space \(dv\) is given by

\[\begin{equation*}
dU_e = \frac{1}{8\pi k}E^2 dv ,
\end{equation*}\]

where \(E^2=\mathbf{E}\cdot\mathbf{E}\) is the square of the magnitude of the electric field.

This is reminiscent of how waves behave: the energy content of a wave is typically proportional to the square of its amplitude.

We can think of the quantity \(dU_{e}/dv\) as the
*energy density* due to the electric field, i.e., the number of joules
per cubic meter needed in order to create that field. (a) How does this quantity
depend on the components of the field vector, \(E_x\), \(E_y\), and \(E_z\)? (b) Suppose
we have a field with \(E_x\neq0\), \(E_y\)=0, and \(E_z\)=0. What would happen to the
energy density if we reversed the sign of \(E_x\)?

\(\triangleright\) To connect this with our previous calculations, we need to find the charge density on the plates in terms of the voltage we were given. Our previous examples were based on the assumption that the gap between the plates was small compared to the size of the plates. Is this valid here? Well, if the plates were square, then the area of \(10^{-4}\ \text{m}^2\) would imply that their sides were \(10^{-2}\) m in length. This is indeed very large compared to the gap of \(10^{-5}\) m, so this assumption appears to be valid (unless, perhaps, the plates have some very strange, long and skinny shape).

Based on this assumption, the field is relatively uniform in the whole volume between the plates, so we can use a single symbol, \(E\), to represent its magnitude, and the relation \(E=d V/d x\) is equivalent to \(E=\Delta V/\Delta x=(\text{1.5 V})/(\text{gap})= 1.5\times10^5\ \text{V}/\text{m}\).

Since the field is uniform, we can dispense with the calculus, and replace \(d U_{e} = (1/8\pi k) E^2 d v\) with \(U_{e} = (1/8\pi k) E^2 v\). The volume equals the area multiplied by the gap, so we have

\[\begin{align*}
U_{e} &= (1/8\pi k) E^2(\text{area})(\text{gap})\\
&= \frac{1}{8\pi\times9\ \times10^9\ \text{N}\!\cdot\!\text{m}^2/\text{C}^2}( 1.5\times10^5\ \text{V}/\text{m})^2(10^{-4}\ \text{m}^2)(10^{-5}\ \text{m})\\
&= 1\times10^{-10}\ \text{J}
\end{align*}\]

Show that the units in the preceding example really do work out to be joules.

(answer in the back of the PDF version of the book)It may also seem strange that the constant \(k\) is in the denominator of the equation \(d U_{e} = (1/8\pi k) E^2 d v\). The Coulomb constant \(k\) tells us how strong electric forces are, so shouldn't it be on top? No. Consider, for instance, an alternative universe in which electric forces are twice as strong as in ours. The numerical value of \(k\) is doubled. Because \(k\) is doubled, all the electric field strengths are doubled as well, which quadruples the quantity \(E^2\). In the expression \(E^2/8\pi k\), we've quadrupled something on top and doubled something on the bottom, which makes the energy twice as big. That makes perfect sense.

According to our old approach, electrical energy is lost because the electric force did positive work as it brought the charges together. (This makes sense because as they come together and accelerate it is their electrical energy that is being lost and converted to kinetic energy.)

By the new method, we must ask how the energy stored in the electric field has changed. In the region indicated approximately by the shading in the figure, the superposing fields of the two charges undergo partial cancellation because they are in opposing directions. The energy in the shaded region is reduced by this effect. In the unshaded region, the fields reinforce, and the energy is increased.

It would be quite a project to do an actual numerical calculation of the energy gained and lost in the two regions (this is a case where the old method of finding energy gives greater ease of computation), but it is fairly easy to convince oneself that the energy is less when the charges are closer. This is because bringing the charges together shrinks the high-energy unshaded region and enlarges the low-energy shaded region.

\(\triangleright\)
On page 102, I proved that for
*gravitational* forces, the interaction of a spherical
shell of mass with other masses outside it is the same as
if the shell's mass was concentrated at its center. On the
interior of such a shell, the forces cancel out exactly.
Since gravity and the electric force both vary as \(1/ r^2\),
the same proof carries over immediately to electrical forces. The magnitude of the outward
electric field contributed by the charge \(+ q\) of the central sphere
is therefore

\[\begin{equation*}
|\mathbf{E}_+| = \left\{
\begin{array}{lr}
0, & r\lt a \\
kq/ r^2, & r> a
\end{array}
\right. ,
\end{equation*}\]

where \(r\) is the distance from the center. Similarly, the magnitude of the
*inward* field contributed
by the outside sphere is

\[\begin{equation*}
|\mathbf{E}_-| = \left\{
\begin{array}{lr}
0, & r\lt b \\
kq/ r^2, & r> b
\end{array}
\right. .
\end{equation*}\]

In the region outside the whole capacitor, the two fields are equal in magnitude, but opposite in direction, so they cancel. We then have for the total field

\[\begin{equation*}
|\mathbf{E}| = \left\{
\begin{array}{lr}
0, & r\lt a \\
kq/ r^2, & a\lt r\lt b \\
0, & r> b
\end{array}
\right. ,
\end{equation*}\]

so to calculate the energy, we only need to worry about the region \(a\lt r\lt b\). The energy density in this region is

\[\begin{align*}
\frac{d U_{e}}{d v} &= \frac{1}{8\pi k} E^2 \\
&= \frac{ kq^2}{8\pi} r^{-4} .
\end{align*}\]

This expression only depends on \(r\), so the energy density is constant across any sphere of radius \(r\). We can slice the region \(a\lt r\lt b\) into concentric spherical layers, like an onion, and the energy within one such layer, extending from \(r\) to \(r+dr\) is

\[\begin{align*}
d U_{e} &= \frac{d U_{e}}{d v} dv \\
&= \frac{d U_{e}}{d v} (\text{area of shell}) (\text{thickness of shell}) \\
&= (\frac{ kq^2}{8\pi} r^{-4}) (4\pi r^2) (dr) \\
&= \frac{ kq^2}{2} r^{-2}dr .
\end{align*}\]

Integrating over all the layers to find the total energy, we have

\[\begin{align*}
U_{e} &= \int d U_{e} \\
&= \int_{a}^{b} \frac{ kq^2}{2} r^{-2}dr \\
&= \left.-\frac{ kq^2}{2} r^{-1}\right|_{a}^{b} \\
&= \frac{ kq^2}{2}\left(\frac{1}{a}-\frac{1}{b}\right) \\
\end{align*}\]

◊

The figure shows a positive charge in the gap between two capacitor plates. Compare the energy of the electric fields in the two cases. Does this agree with what you would have expected based on your knowledge of electrical forces?

◊

The figure shows a spherical capacitor. In the text, the energy stored in its electric field is shown to be

\[\begin{equation*}
U_{e} = \frac{ kq^2}{2}\left(\frac{1}{a}-\frac{1}{b}\right) . \\
\end{equation*}\]

What happens if the difference between \(b\) and \(a\) is very small? Does this make sense in terms of the mechanical work needed in order to separate the charges? Does it make sense in terms of the energy stored in the electric field? Should these two energies be added together?

Similarly, discuss the cases of \(b\rightarrow\infty\) and \(a\rightarrow0\).

◊

Criticize the following statement: “A solenoid makes a charge in the space surrounding it, which dissipates when you release the energy.”

◊

In example 16 on page 587, I argued that for the charges shown in the figure, the fields contain less energy when the charges are closer together, because the region of cancellation expanded, while the region of reinforcing fields shrank. Perhaps a simpler approach is to consider the two extreme possibilities: the case where the charges are infinitely far apart, and the one in which they are at zero distance from each other, i.e., right on top of each other. Carry out this reasoning for the case of (1) a positive charge and a negative charge of equal magnitude, (2) two positive charges of equal magnitude, (3) the gravitational energy of two equal masses.

Example B depended on the close analogy between electric and gravitational
forces. In fact, every argument, proof, and example discussed so far in this section is equally
valid as a gravitational example, provided we take into account one fact: only positive mass
exists, and the gravitational force between two masses is attractive. This is the opposite of
what happens with electrical forces, which are repulsive in the case of two positive charges.
As a consequence of this, we need to assign a *negative* energy density to the gravitational
field! For a gravitational field, we have

\[\begin{equation*}
dU_g = -\frac{1}{8\pi G}g^2 dv ,
\end{equation*}\]

where \(g^2=\mathbf{g}\cdot\mathbf{g}\) is the square of the magnitude of the gravitational field.

So far we've only touched in passing on the topic of magnetic fields, which
will deal with in detail in chapter 11. Magnetism is an interaction between
moving charge and moving charge, i.e., between currents and currents. Since a current
has a direction in space,^{2}
while charge doesn't, we can anticipate that the mathematical rule connecting
a magnetic field to its source-currents will have to be completely different from
the one relating the electric field to its source-charges. However, if you look carefully
at the argument leading to the relation \(dU_e/dv = E^2/8\pi k\), you'll see that
these mathematical details were only necessary to the part of the argument in which
we fixed the constant of proportionality. To establish \(dU_e/dv \propto E^2\),
we only had to use three simple facts:

- The field is proportional to the source.
- Forces are proportional to fields.
- Field contributed by multiple sources add like vectors.

All three of these statements are true for the magnetic field as well, so without knowing anything more specific about magnetic fields --- not even what units are used to measure them! --- we can state with certainty that the energy density in the magnetic field is proportional to the square of the magnitude of the magnetic field. The constant of proportionality is given on p. 667.

The long road leading from the light bulb to the computer
started with one very important step: the introduction of
feedback into electronic circuits. Although the principle of
feedback has been understood and and applied to mechanical
systems for centuries, and to electrical ones since the
early twentieth century, for most of us the word evokes an
image of Jimi Hendrix (or some more recent guitar hero)
intentionally creating earsplitting screeches, or of the
school principal doing the same inadvertently in the
auditorium. In the guitar example, the musician stands in
front of the amp and turns it up so high that the sound
waves coming from the speaker come back to the guitar string
and make it shake harder. This is an example of *positive*
feedback: the harder the string vibrates, the stronger the
sound waves, and the stronger the sound waves, the harder
the string vibrates. The only limit is the power-handling
ability of the amplifier.

Negative feedback is equally important. Your thermostat, for example, provides negative feedback by kicking the heater off when the house gets warm enough, and by firing it up again when it gets too cold. This causes the house's temperature to oscillate back and forth within a certain range. Just as out-of-control exponential freak-outs are a characteristic behavior of positive-feedback systems, oscillation is typical in cases of negative feedback. You have already studied negative feedback extensively in section 3.3 in the case of a mechanical system, although we didn't call it that.

In a mechanical oscillation, energy is exchanged repetitively between potential and kinetic forms, and may also be siphoned off in the form of heat dissipated by friction. In an electrical circuit, resistors are the circuit elements that dissipate heat. What are the electrical analogs of storing and releasing the potential and kinetic energy of a vibrating object? When you think of energy storage in an electrical circuit, you are likely to imagine a battery, but even rechargeable batteries can only go through 10 or 100 cycles before they wear out. In addition, batteries are not able to exchange energy on a short enough time scale for most applications. The circuit in a musical synthesizer may be called upon to oscillate thousands of times a second, and your microwave oven operates at gigahertz frequencies. Instead of batteries, we generally use capacitors and inductors to store energy in oscillating circuits. Capacitors, which you've already encountered, store energy in electric fields. An inductor does the same with magnetic fields.

A capacitor's energy exists in its surrounding electric fields. It is proportional to the square of the field strength, which is proportional to the charges on the plates. If we assume the plates carry charges that are the same in magnitude, \(+q\) and \(-q\), then the energy stored in the capacitor must be proportional to \(q^2\). For historical reasons, we write the constant of proportionality as \(1/2C\),

\[\begin{equation*}
U_C = \frac{1}{2C}q^2 .
\end{equation*}\]

The constant \(C\) is a geometrical property of the capacitor, called its capacitance.

Based on this definition, the units of capacitance must be coulombs squared per joule, and this combination is more conveniently abbreviated as the farad, \(1\ \text{F}=1\ \text{C}^2/\text{J}\). “Condenser” is a less formal term for a capacitor. Note that the labels printed on capacitors often use MF to mean \(\mu\text{F}\), even though MF should really be the symbol for megafarads, not microfarads. Confusion doesn't result from this nonstandard notation, since picofarad and microfarad values are the most common, and it wasn't until the 1990's that even millifarad and farad values became available in practical physical sizes. Figure a shows the symbol used in schematics to represent a capacitor.

\(\triangleright\) Since the plates are metal, the charges on each plate are free to move, and will tend to cluster themselves more densely near the edges due to the mutual repulsion of the other charges in the same plate. However, it turns out that if the gap is small, this is a small effect, so we can get away with assuming uniform charge density on each plate. The result of example 14 then applies, and for the region between the plates, we have \(E=4\pi k\sigma=4\pi kq/ A\) and \(U_{e} = (1/8\pi k) E^2 Ah\). Substituting the first expression into the second, we find \(U_{e}=2\pi kq^2 h/ A\). Comparing this to the definition of capacitance, we end up with \(C= A/4\pi kh\).

Any current will create a magnetic field, so in fact every current-carrying wire in a circuit acts as an inductor! However, this type of “stray” inductance is typically negligible, just as we can usually ignore the stray resistance of our wires and only take into account the actual resistors. To store any appreciable amount of magnetic energy, one usually uses a coil of wire designed specifically to be an inductor. All the loops' contribution to the magnetic field add together to make a stronger field. Unlike capacitors and resistors, practical inductors are easy to make by hand. One can for instance spool some wire around a short wooden dowel. An inductor like this, in the form cylindrical coil of wire, is called a solenoid, c, and a stylized solenoid, d, is the symbol used to represent an inductor in a circuit regardless of its actual geometry.

How much energy does an inductor store? The energy density is proportional to the square of the magnetic field strength, which is in turn proportional to the current flowing through the coiled wire, so the energy stored in the inductor must be proportional to \(I^2\). We write \(L/2\) for the constant of proportionality, giving

\[\begin{equation*}
U_L = \frac{L}{2}I^2 .
\end{equation*}\]

As in the definition of capacitance, we have a
factor of 1/2, which is purely a matter of definition. The
quantity \(L\) is called the *inductance* of the
inductor, and we see that its units must be joules per
ampere squared. This clumsy combination of units is more
commonly abbreviated as the henry, 1 henry = 1 \(\text{J}/\text{A}^2\).
Rather than memorizing this definition, it makes more sense
to derive it when needed from the definition of inductance.
Many people know inductors simply as “coils,” or
“chokes,” and will not understand you if you refer to an
“inductor,” but they will still refer to \(L\) as the
“inductance,” not the “coilance” or “chokeance!”

There is a lumped circuit approximation for inductors, just like the one for capacitors (p. 580). For a capacitor, this means assuming that the electric fields are completely internal, so that components only interact via currents that flow through wires, not due to the physical overlapping of their fields in space. Similarly for an inductor, the lumped circuit approximation is the assumption that the magnetic fields are completely internal.

If two inductors are placed in series, any current that passes through the combined double inductor must pass through both its parts. If we assume the lumped circuit approximation, the two inductors' fields don't interfere with each other, so the energy is doubled for a given current. Thus by the definition of inductance, the inductance is doubled as well. In general, inductances in series add, just like resistances. The same kind of reasoning also shows that the inductance of a solenoid is approximately proportional to its length, assuming the number of turns per unit length is kept constant. (This is only approximately true, because putting two solenoids end-to-end causes the fields just outside their mouths to overlap and add together in a complicated manner. In other words, the lumped-circuit approximation may not be very good.)

When two identical capacitances are placed in parallel, any charge deposited at the terminals of the combined double capacitor will divide itself evenly between the two parts. The electric fields surrounding each capacitor will be half the intensity, and therefore store one quarter the energy. Two capacitors, each storing one quarter the energy, give half the total energy storage. Since capacitance is inversely related to energy storage, this implies that identical capacitances in parallel give double the capacitance. In general, capacitances in parallel add. This is unlike the behavior of inductors and resistors, for which series configurations give addition.

This is consistent with the result of example 18, which had the capacitance of a single parallel-plate capacitor proportional to the area of the plates. If we have two parallel-plate capacitors, and we combine them in parallel and bring them very close together side by side, we have produced a single capacitor with plates of double the area, and it has approximately double the capacitance, subject to any violation of the lumped-circuit approximation due to the interaction of the fields where the edges of the capacitors are joined together.

Inductances in parallel and capacitances in series are explored in homework problems 36 and 33.

Figure h/1 shows the construction of a variable capacitor out of two parallel semicircles of metal. One plate is fixed, while the other can be rotated about their common axis with a knob. The opposite charges on the two plates are attracted to one another, and therefore tend to gather in the overlapping area. This overlapping area, then, is the only area that effectively contributes to the capacitance, and turning the knob changes the capacitance. The simple design can only provide very small capacitance values, so in practice one usually uses a bank of capacitors, wired in parallel, with all the moving parts on the same shaft.

◊

Suppose that two parallel-plate capacitors are wired in parallel, and are placed very close together, side by side, so that the lumped circuit approximation is not very accurate. Will the resulting capacitance be too small, or too big? Could you twist the circuit into a different shape and make the effect be the other way around, or make the effect vanish? How about the case of two inductors in series?

◊

Most practical capacitors do not have an air gap or vacuum gap between the plates; instead, they have an insulating substance called a dielectric. We can think of the molecules in this substance as dipoles that are free to rotate (at least a little), but that are not free to move around, since it is a solid. The figure shows a highly stylized and unrealistic way of visualizing this. We imagine that all the dipoles are intially turned sideways, (1), and that as the capacitor is charged, they all respond by turning through a certain angle, (2). (In reality, the scene might be much more random, and the alignment effect much weaker.)

For simplicity, imagine inserting just one electric dipole into the vacuum gap. For a given amount of charge on the plates, how does this affect the amount of energy stored in the electric field? How does this affect the capacitance?

Now redo the analysis in terms of the mechanical work needed in order to charge up the plates.

Figure j shows the simplest possible oscillating circuit. For any useful application it would actually need to include more components. For example, if it was a radio tuner, it would need to be connected to an antenna and an amplifier. Nevertheless, all the essential physics is there.

We can analyze it without any sweat or tears whatsoever, simply by constructing an analogy with a mechanical system. In a mechanical oscillator, k, we have two forms of stored energy,

\[\begin{align*}
U_{spring} &= \frac{1}{2}kx^2 &(1) \\
K &= \frac{1}{2}mv^2 . &(2)
\end{align*}\]

In the case of a mechanical oscillator, we have usually assumed a friction force of the form that turns out to give the nicest mathematical results, \(F=-bv\). In the circuit, the dissipation of energy into heat occurs via the resistor, with no mechanical force involved, so in order to make the analogy, we need to restate the role of the friction force in terms of energy. The power dissipated by friction equals the mechanical work it does in a time interval \(dt\), divided by \(dt\), \(P=W/dt=Fdx/dt=Fv=-bv^2\), so

\[\begin{equation*}
\text{rate of heat dissipation} = -bv^2 . (3)
\end{equation*}\]

Equation (1) has \(x\) squared, and equations (2) and (3) have \(v\) squared. Because they're squared, the results don't depend on whether these variables are positive or negative. Does this make physical sense?

(answer in the back of the PDF version of the book)In the circuit, the stored forms of energy are

\[\begin{align*}
U_C &= \frac{1}{2C}q^2 &(1') \\
U_L &= \frac{1}{2}LI^2 , &(2')
\end{align*}\]

and the rate of heat dissipation in the resistor is

\[\begin{equation*}
\text{rate of heat dissipation} = -RI^2 . (3')
\end{equation*}\]

Comparing the two sets of equations, we first form analogies between quantities that represent the state of the system at some moment in time:

\[\begin{align*}
x &\leftrightarrow q\\
v &\leftrightarrow I\\
\end{align*}\]

How is \(v\) related mathematically to \(x\)? How is \(I\) connected to \(q\)? Are the two relationships analogous?

(answer in the back of the PDF version of the book)Next we relate the ones that describe the system's permanent characteristics:

\[\begin{align*}
k &\leftrightarrow 1/C\\
m &\leftrightarrow L\\
b &\leftrightarrow R\\
\end{align*}\]

Since the mechanical
system naturally oscillates with a frequency^{3}
\(\omega\approx\sqrt{k/m}\) , we can immediately solve the
electrical version by analogy, giving

\[\begin{equation*}
\omega \approx \frac{1}{\sqrt{LC}} .
\end{equation*}\]

Since the resistance \(R\) is analogous to \(b\) in the mechanical case, we find that the \(Q\) (quality factor, not charge) of the resonance is inversely proportional to \(R\), and the width of the resonance is directly proportional to \(R\).

A radio receiver uses this kind of circuit to pick out the desired station. Since the receiver resonates at a particular frequency, stations whose frequencies are far off will not excite any response in the circuit. The value of \(R\) has to be small enough so that only one station at a time is picked up, but big enough so that the tuner isn't too touchy. The resonant frequency can be tuned by adjusting either \(L\) or \(C\), but variable capacitors are easier to build than variable inductors.

The phone company sends more than one conversation at a time over the same wire, which is accomplished by shifting each voice signal into different range of frequencies during transmission. The number of signals per wire can be maximized by making each range of frequencies (known as a bandwidth) as small as possible. It turns out that only a relatively narrow range of frequencies is necessary in order to make a human voice intelligible, so the phone company filters out all the extreme highs and lows. (This is why your phone voice sounds different from your normal voice.)

\(\triangleright\) If the filter consists of an LRC circuit with a broad resonance centered around 1.0 kHz, and the capacitor is 1 \(\mu\text{F}\) (microfarad), what inductance value must be used?

\(\triangleright\) Solving for \(L\), we have

\[\begin{align*}
L &= \frac{1}{ C\omega^2} \\
&= \frac{1}{(10^{-6}\ \text{F})(2\pi\times10^3\ \text{s}^{-1})^2} \\
&= 2.5\times10^{-3}\ \text{F}^{-1}\text{s}^2
\end{align*}\]

Checking that these really are the same units as henries is a little tedious, but it builds character:

\[\begin{align*}
\text{F}^{-1}\text{s}^2 &= (\text{C}^2/\text{J})^{-1}\text{s}^2 \\
&= \text{J}\cdot\text{C}^{-2}\text{s}^2 \\
&= \text{J}/\text{A}^2 \\
&= \text{H}
\end{align*}\]

The result is 25 mH (millihenries).

This is actually quite a large inductance value, and would require a big, heavy, expensive coil. In fact, there is a trick for making this kind of circuit small and cheap. There is a kind of silicon chip called an op-amp, which, among other things, can be used to simulate the behavior of an inductor. The main limitation of the op-amp is that it is restricted to low-power applications.

What is physically happening in one of these oscillating circuits? Let's first look at the mechanical case, and then draw the analogy to the circuit. For simplicity, let's ignore the existence of damping, so there is no friction in the mechanical oscillator, and no resistance in the electrical one.

Suppose we take the mechanical oscillator and pull the mass away from equilibrium, then release it. Since friction tends to resist the spring's force, we might naively expect that having zero friction would allow the mass to leap instantaneously to the equilibrium position. This can't happen, however, because the mass would have to have infinite velocity in order to make such an instantaneous leap. Infinite velocity would require infinite kinetic energy, but the only kind of energy that is available for conversion to kinetic is the energy stored in the spring, and that is finite, not infinite. At each step on its way back to equilibrium, the mass's velocity is controlled exactly by the amount of the spring's energy that has so far been converted into kinetic energy. After the mass reaches equilibrium, it overshoots due to its own momentum. It performs identical oscillations on both sides of equilibrium, and it never loses amplitude because friction is not available to convert mechanical energy into heat.

Now with the electrical oscillator, the analog of position is charge. Pulling the mass away from equilibrium is like depositing charges \(+q\) and \(-q\) on the plates of the capacitor. Since resistance tends to resist the flow of charge, we might imagine that with no friction present, the charge would instantly flow through the inductor (which is, after all, just a piece of wire), and the capacitor would discharge instantly. However, such an instant discharge is impossible, because it would require infinite current for one instant. Infinite current would create infinite magnetic fields surrounding the inductor, and these fields would have infinite energy. Instead, the rate of flow of current is controlled at each instant by the relationship between the amount of energy stored in the magnetic field and the amount of current that must exist in order to have that strong a field. After the capacitor reaches \(q=0\), it overshoots. The circuit has its own kind of electrical “inertia,” because if charge was to stop flowing, there would have to be zero current through the inductor. But the current in the inductor must be related to the amount of energy stored in its magnetic fields. When the capacitor is at \(q=0\), all the circuit's energy is in the inductor, so it must therefore have strong magnetic fields surrounding it and quite a bit of current going through it.

The only thing that might seem spooky here is that we used to speak as if the current in the inductor caused the magnetic field, but now it sounds as if the field causes the current. Actually this is symptomatic of the elusive nature of cause and effect in physics. It's equally valid to think of the cause and effect relationship in either way. This may seem unsatisfying, however, and for example does not really get at the question of what brings about a voltage difference across the resistor (in the case where the resistance is finite); there must be such a voltage difference, because without one, Ohm's law would predict zero current through the resistor.

Voltage, then, is what is really missing from our story so far.

Let's start by studying the voltage across a capacitor. Voltage is electrical potential energy per unit charge, so the voltage difference between the two plates of the capacitor is related to the amount by which its energy would increase if we increased the absolute values of the charges on the plates from \(q\) to \(q+dq\):

\[\begin{align*}
V_C &= (U_{q+dq}-U_q)/dq \\
&= \frac{dU_C}{dq} \\
&= \frac{d}{dq}\left(\frac{1}{2C}q^2\right) \\
&= \frac{q}{C}
\end{align*}\]

Many books
use this as the definition of capacitance. This equation, by
the way, probably explains the historical reason why \(C\) was
defined so that the energy was *inversely* proportional
to \(C\) for a given value of \(C\): the people who invented the
definition were thinking of a capacitor as a device for
storing charge rather than energy, and the amount of charge
stored for a fixed voltage (the charge “capacity”) is
proportional to \(C\).

In the case of an inductor, we know that if there is a steady, constant current flowing through it, then the magnetic field is constant, and so is the amount of energy stored; no energy is being exchanged between the inductor and any other circuit element. But what if the current is changing? The magnetic field is proportional to the current, so a change in one implies a change in the other. For concreteness, let's imagine that the magnetic field and the current are both decreasing. The energy stored in the magnetic field is therefore decreasing, and by conservation of energy, this energy can't just go away --- some other circuit element must be taking energy from the inductor. The simplest example, shown in figure l, is a series circuit consisting of the inductor plus one other circuit element. It doesn't matter what this other circuit element is, so we just call it a black box, but if you like, we can think of it as a resistor, in which case the energy lost by the inductor is being turned into heat by the resistor. The junction rule tells us that both circuit elements have the same current through them, so \(I\) could refer to either one, and likewise the loop rule tells us \(V_{inductor}+V_{black\ box}=0\), so the two voltage drops have the same absolute value, which we can refer to as \(V\). Whatever the black box is, the rate at which it is taking energy from the inductor is given by \(|P|=|IV|\), so

\[\begin{align*}
|IV| &= \left|\frac{dU_L}{dt}\right| \\
&= \left|\frac{d}{dt}\left( \frac{1}{2}LI^2\right) \right| \\
&= \left|LI\frac{dI}{dt}\right| ,\\
\text{or}
|V| &= \left|L\frac{dI}{dt}\right| , \\
\end{align*}\]

which in many books is taken to be the definition of inductance. The direction of the voltage drop (plus or minus sign) is such that the inductor resists the change in current.

There's one very intriguing thing about this result. Suppose, for concreteness, that the black box in figure l is a resistor, and that the inductor's energy is decreasing, and being converted into heat in the resistor. The voltage drop across the resistor indicates that it has an electric field across it, which is driving the current. But where is this electric field coming from? There are no charges anywhere that could be creating it! What we've discovered is one special case of a more general principle, the principle of induction: a changing magnetic field creates an electric field, which is in addition to any electric field created by charges. (The reverse is also true: any electric field that changes over time creates a magnetic field.) Induction forms the basis for such technologies as the generator and the transformer, and ultimately it leads to the existence of light, which is a wave pattern in the electric and magnetic fields. These are all topics for chapter 11, but it's truly remarkable that we could come to this conclusion without yet having learned any details about magnetism.

The cartoons in figure m compares electric fields made by charges, 1, to electric fields made by changing magnetic fields, 2-3. In m/1, two physicists are in a room whose ceiling is positively charged and whose floor is negatively charged. The physicist on the bottom throws a positively charged bowling ball into the curved pipe. The physicist at the top uses a radar gun to measure the speed of the ball as it comes out of the pipe. They find that the ball has slowed down by the time it gets to the top. By measuring the change in the ball's kinetic energy, the two physicists are acting just like a voltmeter. They conclude that the top of the tube is at a higher voltage than the bottom of the pipe. A difference in voltage indicates an electric field, and this field is clearly being caused by the charges in the floor and ceiling.

In m/2, there are no charges anywhere in the room except for the charged bowling ball. Moving charges make magnetic fields, so there is a magnetic field surrounding the helical pipe while the ball is moving through it. A magnetic field has been created where there was none before, and that field has energy. Where could the energy have come from? It can only have come from the ball itself, so the ball must be losing kinetic energy. The two physicists working together are again acting as a voltmeter, and again they conclude that there is a voltage difference between the top and bottom of the pipe. This indicates an electric field, but this electric field can't have been created by any charges, because there aren't any in the room. This electric field was created by the change in the magnetic field.

The bottom physicist keeps on throwing balls into the pipe, until the pipe is full of balls, m/3, and finally a steady current is established. While the pipe was filling up with balls, the energy in the magnetic field was steadily increasing, and that energy was being stolen from the balls' kinetic energy. But once a steady current is established, the energy in the magnetic field is no longer changing. The balls no longer have to give up energy in order to build up the field, and the physicist at the top finds that the balls are exiting the pipe at full speed again. There is no voltage difference any more. Although there is a current, \(dI/dt\) is zero.

The simplest solution is to connect an inductor, known as the “ballast,” in series with the tube, and run the whole thing on an AC voltage. During each cycle, as the voltage reaches the point where the chain reaction begins, there is a surge of current, but the inductor resists such a sudden change of current, and the energy that would otherwise have burned out the bulb is instead channeled into building a magnetic field.

A common household fluorescent lightbulb consists of a gas discharge tube in which the glass is coated with a fluorescent material. The gas in the tube emits ultraviolet light, which is absorbed by the coating, and the coating then glows in the visible spectrum.

Until recently, it was common for a fluroescent light's ballast to be a simple inductor, and for the whole device to be operated at the 60 Hz frequency of the electrical power lines. This caused the lights to flicker annoyingly at 120 Hz, and could also cause an audible hum, since the magnetic field surrounding the inductor could exert mechanical forces on things. These days, the trend is toward using a solid-state circuit that mimics the behavior of an inductor, but at a frequency in the kilohertz range, eliminating the flicker and hum. Modern compact fluorescent bulbs electronic have ballasts built into their bases, so they can be used as plug-in replacements for incandescent bulbs. A compact fluorescent bulb uses about 1/4 the electricity of an incandescent bulb, lasts ten times longer, and saves $30 worth of electricity over its lifetime.

◊

What happens when the physicist at the bottom in figure m/3 starts getting tired, and decreases the current?

Up until now I've soft-pedaled the fact that by changing the characteristics of an oscillator, it is possible to produce non-oscillatory behavior. For example, imagine taking the mass-on-a-spring system and making the spring weaker and weaker. In the limit of small \(k\), it's as though there was no spring whatsoever, and the behavior of the system is that if you kick the mass, it simply starts slowing down. For friction proportional to \(v\), as we've been assuming, the result is that the velocity approaches zero, but never actually reaches zero. This is unrealistic for the mechanical oscillator, which will not have vanishing friction at low velocities, but it is quite realistic in the case of an electrical circuit, for which the voltage drop across the resistor really does approach zero as the current approaches zero.

We do not even have to reduce \(k\) to exactly zero in order to get non-oscillatory behavior. There is actually a finite, critical value below which the behavior changes, so that the mass never even makes it through one cycle. This is the case of overdamping, discussed on page 186.

Electrical circuits can exhibit all the same behavior. For simplicity we will analyze only the cases of LRC circuits with \(L=0\) or \(C=0\).

We first analyze the RC circuit, o. In reality one would have to “kick” the circuit, for example by briefly inserting a battery, in order to get any interesting behavior. We start with Ohm's law and the equation for the voltage across a capacitor:

\[\begin{align*}
V_R &= IR \\
V_C &= q/C
\end{align*}\]

The loop rule tells us

\[\begin{equation*}
V_R + V_C = 0 ,
\end{equation*}\]

and combining the three equations results in a relationship between \(q\) and \(I\):

\[\begin{equation*}
I = -\frac{1}{RC}q
\end{equation*}\]

The negative sign tells us that the current tends to reduce the charge on the capacitor, i.e., to discharge it. It makes sense that the current is proportional to \(q\) : if \(q\) is large, then the attractive forces between the \(+q\) and \(-q\) charges on the plates of the capacitor are large, and charges will flow more quickly through the resistor in order to reunite. If there was zero charge on the capacitor plates, there would be no reason for current to flow. Since amperes, the unit of current, are the same as coulombs per second, it appears that the quantity \(RC\) must have units of seconds, and you can check for yourself that this is correct. \(RC\) is therefore referred to as the time constant of the circuit.

How exactly do \(I\) and \(q\) vary with time? Rewriting \(I\) as \(dq/dt\), we have

\[\begin{equation*}
\frac{dq}{dt} = -\frac{1}{RC}q .
\end{equation*}\]

We need a function \(q(t)\) whose derivative equals itself, but multiplied by a negative constant. A function of the form \(ae^t\), where \(e=2.718...\) is the base of natural logarithms, is the only one that has its derivative equal to itself, and \(ae^{bt}\) has its derivative equal to itself multiplied by \(b\). Thus our solution is

\[\begin{equation*}
q = q_\text{o}\exp\left(-\frac{t}{RC}\right) .
\end{equation*}\]

The RL circuit, q, can be attacked by similar methods, and it can easily be shown that it gives

\[\begin{equation*}
I = I_\text{o}\exp\left(-\frac{R}{L}t\right) .
\end{equation*}\]

The RL time constant equals \(L/R\).

When we suddenly break an RL circuit, what will happen? It might seem that we're faced with a paradox, since we only have two forms of energy, magnetic energy and heat, and if the current stops suddenly, the magnetic field must collapse suddenly. But where does the lost magnetic energy go? It can't go into resistive heating of the resistor, because the circuit has now been broken, and current can't flow!

The way out of this conundrum is to recognize that the open gap in the circuit has a resistance which is large, but not infinite. This large resistance causes the RL time constant \(L/ R\) to be very small. The current thus continues to flow for a very brief time, and flows straight across the air gap where the circuit has been opened. In other words, there is a spark!

We can determine based on several different lines of reasoning that the voltage drop from one end of the spark to the other must be very large. First, the air's resistance is large, so \(V= IR\) requires a large voltage. We can also reason that all the energy in the magnetic field is being dissipated in a short time, so the power dissipated in the spark, \(P= IV\), is large, and this requires a large value of \(V\). (\(I\) isn't large --- it is decreasing from its initial value.) Yet a third way to reach the same result is to consider the equation \(V_{L}=dI/dt\) : since the time constant is short, the time derivative \(dI/dt\) is large.

This is exactly how a car's spark plugs work. Another application is to electrical safety: it can be dangerous to break an inductive circuit suddenly, because so much energy is released in a short time. There is also no guarantee that the spark will discharge across the air gap; it might go through your body instead, since your body might have a lower resistance.

◊

A gopher gnaws through one of the wires in the DC lighting system in your front yard, and the lights turn off. At the instant when the circuit becomes open, we can consider the bare ends of the wire to be like the plates of a capacitor, with an air gap (or gopher gap) between them. What kind of capacitance value are we talking about here? What would this tell you about the \(RC\) time constant?

For a more detailed treatment of complex numbers, see ch. 3 of
James Nearing's free book at

http://www.physics.miami.edu/nearing/mathmethods/.

We assume there is a number, \(i\), such that \(i^2=-1\). The square roots of \(-1\) are then \(i\) and \(-i\). (In electrical engineering work, where \(i\) stands for current, \(j\) is sometimes used instead.) This gives rise to a number system, called the complex numbers, containing the real numbers as a subset. Any complex number \(z\) can be written in the form \(z=a+bi\), where \(a\) and \(b\) are real, and \(a\) and \(b\) are then referred to as the real and imaginary parts of \(z\). A number with a zero real part is called an imaginary number. The complex numbers can be visualized as a plane, with the real number line placed horizontally like the \(x\) axis of the familiar \(x-y\) plane, and the imaginary numbers running along the \(y\) axis. The complex numbers are complete in a way that the real numbers aren't: every nonzero complex number has two square roots. For example, 1 is a real number, so it is also a member of the complex numbers, and its square roots are \(-1\) and 1. Likewise, \(-1\) has square roots \(i\) and \(-i\), and the number \(i\) has square roots \(1/\sqrt{2}+i/\sqrt{2}\) and \(-1/\sqrt{2}-i/\sqrt{2}\).

Complex numbers can be added and subtracted by adding or subtracting their real and imaginary parts. Geometrically, this is the same as vector addition.

The complex numbers \(a+bi\) and \(a-bi\), lying at equal distances above and below the real axis, are called complex conjugates. The results of the quadratic formula are either both real, or complex conjugates of each other. The complex conjugate of a number \(z\) is notated as \(\bar{z}\) or \(z^*\).

The complex numbers obey all the same rules of arithmetic as the reals, except that they can't be ordered along a single line. That is, it's not possible to say whether one complex number is greater than another. We can compare them in terms of their magnitudes (their distances from the origin), but two distinct complex numbers may have the same magnitude, so, for example, we can't say whether \(1\) is greater than \(i\) or \(i\) is greater than \(1\).

\(\triangleright\) Our proof can use any ordinary rules of arithmetic, except for ordering.

\[\begin{align*}
(\frac{1}{\sqrt{2}}+\frac{i}{\sqrt{2}})^2
& = \frac{1}{\sqrt{2}}\cdot\frac{1}{\sqrt{2}}
+\frac{1}{\sqrt{2}}\cdot\frac{i}{\sqrt{2}}
+\frac{i}{\sqrt{2}}\cdot\frac{1}{\sqrt{2}}
+\frac{i}{\sqrt{2}}\cdot\frac{i}{\sqrt{2}} \\
&= \frac{1}{2}(1+i+i-1) \\
&= i
\end{align*}\]

Example 27 showed one method of multiplying complex numbers. However, there is another nice interpretation of complex multiplication. We define the argument of a complex number as its angle in the complex plane, measured counterclockwise from the positive real axis. Multiplying two complex numbers then corresponds to multiplying their magnitudes, and adding their arguments.

Using this interpretation of multiplication, how could you find the square roots of a complex number?

(answer in the back of the PDF version of the book)This whole system was built up in order to make every number have square roots. What about cube roots, fourth roots, and so on? Does it get even more weird when you want to do those as well? No. The complex number system we've already discussed is sufficient to handle all of them. The nicest way of thinking about it is in terms of roots of polynomials. In the real number system, the polynomial \(x^2-1\) has two roots, i.e., two values of \(x\) (plus and minus one) that we can plug in to the polynomial and get zero. Because it has these two real roots, we can rewrite the polynomial as \((x-1)(x+1)\). However, the polynomial \(x^2+1\) has no real roots. It's ugly that in the real number system, some second-order polynomials have two roots, and can be factored, while others can't. In the complex number system, they all can. For instance, \(x^2+1\) has roots \(i\) and \(-i\), and can be factored as \((x-i)(x+i)\). In general, the fundamental theorem of algebra states that in the complex number system, any nth-order polynomial can be factored completely into \(n\) linear factors, and we can also say that it has \(n\) complex roots, with the understanding that some of the roots may be the same. For instance, the fourth-order polynomial \(x^4+x^2\) can be factored as \((x-i)(x+i)(x-0)(x-0)\), and we say that it has four roots, \(i\), \(-i\), 0, and 0, two of which happen to be the same. This is a sensible way to think about it, because in real life, numbers are always approximations anyway, and if we make tiny, random changes to the coefficients of this polynomial, it will have four distinct roots, of which two just happen to be very close to zero.

◊

Find \(\arg i\), \(\arg(-i)\), and \(\arg 37\), where \(\arg z\) denotes the argument of the complex number \(z\).

◊

Visualize the following multiplications in the complex plane using the interpretation of multiplication in terms of multiplying magnitudes and adding arguments: \((i)(i)=-1\), \((i)(-i)=1\), \((-i)(-i)=-1\).

◊

If we visualize \(z\) as a point in the complex plane, how should we visualize \(-z\)? What does this mean in terms of arguments? Give similar interpretations for \(z^2\) and \(\sqrt{z}\).

◊

Find four different complex numbers \(z\) such that \(z^4=1\).

◊

Compute the following. Use the magnitude and argument, not the real and imaginary parts.

\[\begin{equation*}
|1+i| ,
\arg(1+i) ,
\left|\frac{1}{1+i}\right| ,
\arg\left(\frac{1}{1+i}\right) ,
\end{equation*}\]

Based on the results above, compute the real and imaginary parts of \(1/(1+i)\).

Having expanded our horizons to include the complex numbers, it's natural to want to extend functions we knew and loved from the world of real numbers so that they can also operate on complex numbers. The only really natural way to do this in general is to use Taylor series. A particularly beautiful thing happens with the functions \(e^x\), \(\sin x\), and \(\cos x\):

\[\begin{align*}
e^x &= 1 + \frac{1}{2!}x^2 + \frac{1}{3!}x^3 + ... \\
\cos x &= 1 - \frac{1}{2!}x^2 + \frac{1}{4!}x^4 - ... \\
\sin x &= x - \frac{1}{3!}x^3 + \frac{1}{5!}x^5 - ...
\end{align*}\]

If \(x=i\phi\) is an imaginary number, we have

\[\begin{equation*}
e^{i\phi} = \cos \phi + i \sin \phi ,
\end{equation*}\]

a result known as Euler's formula. The geometrical interpretation in the complex plane is shown in figure x.

Although the result may seem like something out of a freak show at first, applying the definition of the exponential function makes it clear how natural it is:

\[\begin{align*}
e^x = \lim_{n\rightarrow \infty} \left(1+\frac{x}{n}\right)^n .
\end{align*}\]

When \(x=i\phi\) is imaginary, the quantity \((1+i\phi/n)\) represents a number lying just above 1 in the complex plane. For large \(n\), \((1+i\phi/n)\) becomes very close to the unit circle, and its argument is the small angle \(\phi/n\). Raising this number to the nth power multiplies its argument by \(n\), giving a number with an argument of \(\phi\).

Euler's formula is used frequently in physics and engineering.

\(\triangleright\) Write the sine and cosine functions in terms of exponentials.

\(\triangleright\) Euler's formula for \(x=-i\phi\) gives \(\cos \phi - i \sin \phi\), since \(\cos(-\theta)=\cos\theta\), and \(\sin(-\theta)=-\sin\theta\).

\[\begin{align*}
\cos x &= \frac{e^{ix}+e^{-ix}}{2} \\
\sin x &= \frac{e^{ix}-e^{-ix}}{2i}
\end{align*}\]

\(\triangleright\) Evaluate

\[\begin{equation*}
\int e^x \cos x dx
\end{equation*}\]

\(\triangleright\) This seemingly impossible integral becomes easy if we rewrite the cosine in terms of exponentials:

\[\begin{align*}
\int e^x & \cos x dx \\
&= \int e^x \left(\frac{e^{ix}+e^{-ix}}{2}\right) dx \\
&= \frac{1}{2} \int (e^{(1+i)x}+e^{(1-i)x})dx \\
&= \frac{1}{2} \left( \frac{e^{(1+i)x}}{1+i}+\frac{e^{(1-i)x}}{1-i} \right)+ c
\end{align*}\]

Since this result is the integral of a real-valued function, we'd like it to be
real, and in fact it is, since the first and second terms are complex conjugates of
one another. If we wanted to, we could use Euler's theorem to convert it back to
a manifestly real result.^{5}

So far we have been thinking in terms of the free oscillations of a circuit. This is like a mechanical oscillator that has been kicked but then left to oscillate on its own without any external force to keep the vibrations from dying out. Suppose an LRC circuit is driven with a sinusoidally varying voltage, such as will occur when a radio tuner is hooked up to a receiving antenna. We know that a current will flow in the circuit, and we know that there will be resonant behavior, but it is not necessarily simple to relate current to voltage in the most general case. Let's start instead with the special cases of LRC circuits consisting of only a resistance, only a capacitance, or only an inductance. We are interested only in the steady-state response.

The purely resistive case is easy. Ohm's law gives

\[\begin{equation*}
I = \frac{V}{R} .
\end{equation*}\]

In the purely capacitive case, the relation \(V=q/C\) lets us calculate

\[\begin{align*}
I &= \frac{dq}{dt} \\
&= C \frac{dV}{dt} .
\end{align*}\]

This is partly analogous to Ohm's law. For example, if we double the amplitude of a sinusoidally varying AC voltage, the derivative \(dV/dt\) will also double, and the amplitude of the sinusoidally varying current will also double. However, it is not true that \(I=V/R\), because taking the derivative of a sinusoidal function shifts its phase by 90 degrees. If the voltage varies as, for example, \(V(t)=V_\text{o}\sin (\omega t)\), then the current will be \(I(t)=\omega C V_\text{o}\cos (\omega t)\). The amplitude of the current is \(\omega C V_\text{o}\), which is proportional to \(V_\text{o}\), but it's not true that \(I(t)=V(t)/R\) for some constant \(R\).

A second problem that crops up is that our entire analysis of DC resistive circuits was built on the foundation of the loop rule and the junction rule, both of which are statements about sums. To apply the junction rule to an AC circuit, for exampe, we would say that the sum of the sine waves describing the currents coming into the junction is equal (at every moment in time) to the sum of the sine waves going out. Now sinusoidal functions have a remarkable property, which is that if you add two different sinusoidal functions having the same frequency, the result is also a sinusoid with that frequency. For example, \(\cos\omega t+\sin\omega t=\sqrt{2}\sin(\omega t+\pi/4)\), which can be proved using trig identities. The trig identities can get very cumbersome, however, and there is a much easier technique involving complex numbers.

Figure aa shows a useful way to visualize what's going on. When a circuit is oscillating at a frequency \(\omega\), we use points in the plane to represent sinusoidal functions with various phases and amplitudes.

Which of the following functions can be represented in this way? \(\cos(6t-4)\), \(\cos^2t\), \(\tan t\)

(answer in the back of the PDF version of the book)The simplest examples of how to visualize this in polar coordinates are ones like \(\cos \omega t+\cos \omega t=2\cos \omega t\), where everything has the same phase, so all the points lie along a single line in the polar plot, and addition is just like adding numbers on the number line. The less trivial example \(\cos\omega t+\sin\omega t=\sqrt{2}\sin(\omega t+\pi/4)\), can be visualized as in figure ab.

Figure ab suggests that all of this can be tied together nicely if we identify our plane with the plane of complex numbers. For example, the complex numbers 1 and \(i\) represent the functions \(\sin\omega t\) and \(\cos\omega t\). In figure z, for example, the voltage across the capacitor is a sine wave multiplied by a number that gives its amplitude, so we associate that function with a number \(\tilde{V}\) lying on the real axis. Its magnitude, \(|\tilde{V}|\), gives the amplitude in units of volts, while its argument \(\arg \tilde{V}\), gives its phase angle, which is zero. The current is a multiple of a sine wave, so we identify it with a number \(\tilde{I}\) lying on the imaginary axis. We have \(\arg\tilde{I}=90°\), and \(|\tilde{I}|\) is the amplitude of the current, in units of amperes. But comparing with our result above, we have \(|\tilde{I}|=\omega C|\tilde{V}|\). Bringing together the phase and magnitude information, we have \(\tilde{I}=i\omega C\tilde{V}\). This looks very much like Ohm's law, so we write

\[\begin{equation*}
\tilde{I} = \frac{\tilde{V}}{Z_C} ,
\end{equation*}\]

where the quantity

\[\begin{equation*}
Z_C = -\frac{i}{\omega C} , \text{[impedance of a capacitor]}
\end{equation*}\]

having units of ohms, is called the *impedance* of
the capacitor at this frequency.

It makes sense that the impedance becomes infinite at zero frequency. Zero frequency means that it would take an infinite time before the voltage would change by any amount. In other words, this is like a situation where the capacitor has been connected across the terminals of a battery and been allowed to settle down to a state where there is constant charge on both terminals. Since the electric fields between the plates are constant, there is no energy being added to or taken out of the field. A capacitor that can't exchange energy with any other circuit component is nothing more than a broken (open) circuit.

Note that we have two types of complex numbers: those that represent sinusoidal functions of time, and those that represent impedances. The ones that represent sinusoidal functions have tildes on top, which look like little sine waves.

Why can't a capacitor have its impedance printed on it along with its capacitance?

(answer in the back of the PDF version of the book)Similar math (but this time with an integral instead of a derivative) gives

\[\begin{equation*}
Z_L = i\omega L \text{[impedance of an inductor]}
\end{equation*}\]

for an inductor. It makes sense that the inductor has lower impedance at lower frequencies, since at zero frequency there is no change in the magnetic field over time. No energy is added to or released from the magnetic field, so there are no induction effects, and the inductor acts just like a piece of wire with negligible resistance. The term “choke” for an inductor refers to its ability to “choke out” high frequencies.

The phase relationships shown in figures z and ac can be remembered using my own mnemonic, “eVIL,” which shows that the voltage (V) leads the current (I) in an inductive circuit, while the opposite is true in a capacitive one. A more traditional mnemonic is “ELI the ICE man,” which uses the notation E for emf, a concept closely related to voltage (see p. 688).

Summarizing, the impedances of resistors, capacitors, and inductors are

\[\begin{align*}
Z_R &= R\\
Z_C &= -\frac{i}{\omega C}\\
Z_L &= i\omega L .
\end{align*}\]

An LRC circuit only responds to a certain range (band) of frequencies centered around its resonant frequency. As a filter, this is known as a bandpass filter. If you turn down both the bass and the treble on your stereo, you have created a bandpass filter.

To create a high-pass or low-pass filter, we only need to insert a capacitor or inductor, respectively, in series. For instance, a very basic surge protector for a computer could be constructed by inserting an inductor in series with the computer. The desired 60 Hz power from the wall is relatively low in frequency, while the surges that can damage your computer show much more rapid time variation. Even if the surges are not sinusoidal signals, we can think of a rapid “spike” qualitatively as if it was very high in frequency --- like a high-frequency sine wave, it changes very rapidly.

Inductors tend to be big, heavy, expensive circuit
elements, so a simple surge protector would be more likely
to consist of a capacitor in *parallel* with the
computer. (In fact one would normally just connect one side
of the power circuit to ground via a capacitor.) The
capacitor has a very high impedance at the low frequency of
the desired 60 Hz signal, so it siphons off very little of
the current. But for a high-frequency signal, the capacitor's
impedance is very small, and it acts like a zero-impedance,
easy path into which the current is diverted.

The main things to be careful about with impedance are that (1) the concept only applies to a circuit that is being driven sinusoidally, (2) the impedance of an inductor or capacitor is frequency-dependent.

◊

Figure z on page 609 shows the voltage and current for a capacitor. Sketch the \(q\)-\(t\) graph, and use it to give a physical explanation of the phase relationship between the voltage and current. For example, why is the current zero when the voltage is at a maximum or minimum?

◊

Figure ac on page 611 shows the voltage and current for an inductor. The power is considered to be positive when energy is being put into the inductor's magnetic field. Sketch the graph of the power, and then the graph of \(U\), the energy stored in the magnetic field, and use it to give a physical explanation of the \(P\)-\(t\) graph. In particular, discuss why the frequency is doubled on the \(P\)-\(t\) graph.

◊

Relate the features of the graph in figure ac on page 611 to the story told in cartoons in figure m/2-3 on page 600.

How much power is delivered when an oscillating voltage is applied to an impedance? The equation \(P=IV\) is generally true, since voltage is defined as energy per unit charge, and current is defined as charge per unit time: multiplying them gives energy per unit time. In a DC circuit, all three quantities were constant, but in an oscillating (AC) circuit, all three display time variation.

First let's examine the case of
a resistor. For instance, you're probably reading this book from
a piece of paper illuminated by a glowing lightbulb, which is
driven by an oscillating voltage with amplitude \(V_\text{o}\).
In the special case of a resistor, we know that \(I\) and \(V\) are in phase.
For example, if \(V\) varies as \(V_\text{o}\cos \omega t\), then \(I\) will be a cosine as well,
\(I_\text{o}\cos \omega t\). The power is then \(I_\text{o}V_\text{o}\cos^2\omega t\), which
is always positive,^{6} and varies between 0 and \(I_\text{o}V_\text{o}\).
Even if the time variation was \(\cos\omega t\) or \(\sin(\omega t+\pi/4)\),
we would still have a maximum power of \(I_\text{o}V_\text{o}\), because both the voltage and the
current would reach their maxima at the same time. In a lightbulb, the moment of maximum
power is when the circuit is most rapidly heating the filament. At the
instant when \(P=0\), a quarter of a cycle later, no current is flowing, and no electrical
energy is being turned into heat. Throughout the whole cycle, the filament is getting rid
of energy by radiating light.^{7}
Since the circuit oscillates at a frequency^{8} of \(60\ \text{Hz}\), the temperature doesn't really have time to
cycle up or down very much over the 1/60 s period of the oscillation, and we don't notice
any significant variation in the brightness of the light, even with a short-exposure
photograph.

Thus, what we really want to know is the average power, “average” meaning the average over one full cycle. Since we're covering a whole cycle with our average, it doesn't matter what phase we assume. Let's use a cosine. The total amount of energy transferred over one cycle is

\[\begin{align*}
E &= \int dE \\
&= \int_0^T \frac{dE}{dt} dt , \\
\text{where $T=2\pi/\omega$ is the period.}
E &= \int_0^T P dt \\
&= \int_0^T P dt \\
&= \int_0^T I_\text{o}V_\text{o} \cos^2\omega t dt \\
&= I_\text{o}V_\text{o} \int_0^T \cos^2\omega t dt \\
&= I_\text{o}V_\text{o} \int_0^T \frac{1}{2} \left(1+\cos 2\omega t\right) dt \\
\text{The reason for using the trig identity $\cos^2 x=(1+\cos 2 x)/2$ in the last step is that
it lets us get the answer without doing a hard integral. Over the course of one full
cycle, the quantity $\cos 2\omega t$ goes positive, negative, positive, and negative again,
so the integral of it is zero. We then have}
E &= I_\text{o}V_\text{o} \int_0^T \frac{1}{2} dt \\
&= \frac{I_\text{o}V_\text{o}T}{2}
\end{align*}\]

The average power is

\[\begin{align*}
P_{av} &= \frac{\text{energy transferred in one full cycle}}{\text{time for one full cycle}} \\
&= \frac{I_\text{o}V_\text{o}T/2}{T} \\
&= \frac{I_\text{o}V_\text{o}}{2} ,\\
\end{align*}\]

i.e., the average is half the maximum. The power varies from \(0\) to \(I_\text{o}V_\text{o}\), and it spends equal amounts of time above and below the maximum, so it isn't surprising that the average power is half-way in between zero and the maximum. Summarizing, we have

\[\begin{align*}
P_{av} &= \frac{I_\text{o}V_\text{o}}{2} \text{[average power in a resistor]}\\
\end{align*}\]

for a resistor.

Suppose one day the electric company decided to start supplying your electricity as
DC rather than AC. How would the DC voltage have to be related to the amplitude
\(V_\text{o}\) of the AC voltage previously used if they wanted your lightbulbs to
have the same brightness as before? The resistance of the bulb, \(R\), is a fixed
value, so we need to relate the power to the voltage and the resistance, eliminating
the current. In the DC case, this gives \(P=IV=(V/R)V=V^2/R\). (For DC, \(P\) and \(P_{av}\)
are the same.) In the AC case, \(P_{av} = I_\text{o}V_\text{o}/2=V_\text{o}^2/2R\).
Since there is no factor of 1/2 in the DC case, the same power could be provided
with a DC voltage that was smaller by a factor of \(1/\sqrt{2}\).
Although you will hear people say that household voltage in the U.S. is 110 V,
its amplitude is actually \((110\ \text{V})\times\sqrt{2}\approx160\ \text{V}\). The reason
for referring to \(V_\text{o}/\sqrt{2}\) as “the” voltage is that people who are naive
about AC circuits can plug \(V_\text{o}/\sqrt{2}\) into a familiar DC equation like
\(P=V^2/R\) and get the right *average* answer. The quantity \(V_\text{o}/\sqrt{2}\)
is called the “RMS” voltage,
which stands for “root mean square.” The idea is that if you square the function
\(V(t)\), take its average (mean) over one cycle, and then take the square root of that
average, you get \(V_\text{o}/\sqrt{2}\). Many digital meters provide RMS readouts for
measuring AC voltages and currents.

For a capacitor, the calculation starts out the same, but ends up with a twist. If the voltage varies as a cosine, \(V_\text{o}\cos \omega t\), then the relation \(I=CdV/dt\) tells us that the current will be some constant multiplied by minus the sine, \(-V_\text{o}\sin \omega t\). The integral we did in the case of a resistor now becomes

\[\begin{equation*}
E = \int_0^T -I_\text{o}V_\text{o} \sin \omega t \cos \omega t dt ,\\
\end{equation*}\]

and based on figure ae, you can easily convince yourself that over the course of one full cycle, the power spends two quarter-cycles being negative and two being positive. In other words, the average power is zero!

Why is this? It makes sense if you think in terms of energy. A resistor converts electrical energy to heat, never the other way around. A capacitor, however, merely stores electrical energy in an electric field and then gives it back. For a capacitor,

\[\begin{align*}
P_{av} &= 0 \text{[average power in a capacitor]}\\
\end{align*}\]

Notice that although the average power is zero, the power at any given instant is
*not* typically zero, as shown in figure ae.
The capacitor *does*
transfer energy: it's just that after borrowing some energy, it always pays it
back in the next quarter-cycle.

The analysis for an inductor is similar to that for a capacitor: the power averaged over one cycle is zero. Again, we're merely storing energy temporarily in a field (this time a magnetic field) and getting it back later.

Figure af shows a commonly encountered situation: we wish to maximize the average power, \(P_{av}\), delivered to the load for a fixed value of \(V_\text{o}\), the amplitude of the oscillating driving voltage. We assume that the impedance of the transmission line, \(Z_T\) is a fixed value, over which we have no control, but we are able to design the load, \(Z_\text{o}\), with any impedance we like. For now, we'll also assume that both impedances are resistive. For example, \(Z_T\) could be the resistance of a long extension cord, and \(Z_\text{o}\) could be a lamp at the end of it. The result generalizes immediately, however, to any kind of impedance. For example, the load could be a stereo speaker's magnet coil, which is displays both inductance and resistance. (For a purely inductive or capacitive load, \(P_{av}\) equals zero, so the problem isn't very interesting!)

Since we're assuming both the load and the transmission line are resistive, their impedances add in series, and the amplitude of the current is given by

\[\begin{align*}
I_\text{o} &= \frac{V_\text{o}}{Z_\text{o}+Z_T} ,\\
\text{so}
P_{av} &= I_\text{o}V_\text{o}/2 \\
&= I_\text{o}^2Z_\text{o}/2 \\
&= \frac{V_\text{o}^2Z_\text{o}}{\left(Z_\text{o}+Z_T\right)^2}/2 .
\text{The maximum of this expression occurs where the derivative is zero,}
0 &= \frac{1}{2}\frac{d}{dZ_\text{o}}\left[\frac{V_\text{o}^2Z_\text{o}}{\left(Z_\text{o}+Z_T\right)^2}\right] \\
0 &= \frac{1}{2}\frac{d}{dZ_\text{o}}\left[\frac{Z_\text{o}}{\left(Z_\text{o}+Z_T\right)^2}\right] \\
0 &= \left(Z_\text{o}+Z_T\right)^{-2}-2Z_\text{o}\left(Z_\text{o}+Z_T\right)^{-3} \\
0 &= \left(Z_\text{o}+Z_T\right)-2Z_\text{o} \\
Z_\text{o} &= Z_T
\end{align*}\]

In other words, to maximize the power delivered to the load, we should make the load's impedance the same as the transmission line's. This result may seem surprising at first, but it makes sense if you think about it. If the load's impedance is too high, it's like opening a switch and breaking the circuit; no power is delivered. On the other hand, it doesn't pay to make the load's impedance too small. Making it smaller does give more current, but no matter how small we make it, the current will still be limited by the transmission line's impedance. As the load's impedance approaches zero, the current approaches this fixed value, and the the power delivered, \(I_\text{o}^2Z_\text{o}\), decreases in proportion to \(Z_\text{o}\).

Maximizing the power transmission by matching \(Z_T\) to \(Z_\text{o}\) is called *impedance
matching*. For example, an 8-ohm home stereo speaker will be correctly matched to
a home stereo amplifier with an internal impedance of 8 ohms, and 4-ohm car speakers
will be correctly matched to a car stereo with a 4-ohm internal impedance. You might think
impedance matching would be unimportant because even if, for example, we used a car stereo
to drive 8-ohm speakers, we could compensate for the mismatch simply by turning the volume
knob higher. This is indeed one way to compensate for any impedance mismatch, but there
is always a price to pay. When the impedances are matched, half the power is dissipated
in the transmission line and half in the load. By connecting a 4-ohm amplifier to an
8-ohm speaker, however, you would be setting up a situation in two watts were being dissipated
as heat inside the amp for every amp being delivered to the speaker. In other words, you
would be wasting energy, and perhaps burning out your amp when you turned up the volume to
compensate for the mismatch.

How do impedances combine in series and parallel? The beauty of treating them as complex numbers is that they simply combine according to the same rules you've already learned as resistances.

\(\triangleright\) Impedances in series, like resistances in series, add. The capacitor and inductor act as if they were a single circuit element with an impedance

\[\begin{align*}
Z &= Z_{L}+ Z_{C}\\
&= i\omega L-\frac{ i}{\omega C} .\\
\text{The current is then}
\tilde{ I} = \frac{\tilde{ V}}{ i\omega L- i/\omega C} .
\end{align*}\]

We don't care about the phase of the current, only its amplitude, which is
represented by the absolute value of the complex number \(\tilde{ I}\), and
this can be maximized by making
\(| i\omega L- i/\omega C|\) as small as possible.
But there is some frequency at which this quantity is *zero* ---

\[\begin{gather*}
0 = i\omega L-\frac{ i}{\omega C}\\
\frac{1}{\omega C} = \omega L\\
\omega = \frac{1}{\sqrt{ LC}}
\end{gather*}\]

At this frequency, the current is infinite! What is going on physically? This is an LRC circuit with \(R=0\). It has a resonance at this frequency, and because there is no damping, the response at resonance is infinite. Of course, any real LRC circuit will have some damping, however small (cf. figure j on page 181).

\(\triangleright\) What is the amplitude of the current in a series LRC circuit?

\(\triangleright\) Generalizing from example 32, we add a third, real impedance:

\[\begin{align*}
|\tilde{ I}| &= \frac{|\tilde{ V}|}{| Z|} \\
&= \frac{|\tilde{ V}|}{| R+ i\omega L- i/\omega C|} \\
&= \frac{|\tilde{ V}|}{\sqrt{ R^2+(\omega L-1/\omega C)^2}}
\end{align*}\]

This result would have taken pages of algebra without the complex number technique!

A second-order filter, like ag/2, is one that cuts off more sharply: at high frequencies, the power goes like \(\omega^{-4}\). To analyze this circuit, we first calculate the total impedance:

\[\begin{equation*}
Z = Z_{L}+( Z_{C}^{-1}+ Z_R^{-1})^{-1}
\end{equation*}\]

All the current passes through the inductor, so if the driving voltage being supplied on the left is \(\tilde{ V}_d\), we have

\[\begin{equation*}
\tilde{ V}_d = \tilde{ I}_{L} Z ,
\end{equation*}\]

and we also have

\[\begin{equation*}
\tilde{ V}_{L} = \tilde{ I}_{L} Z_L .
\end{equation*}\]

The loop rule, applied to the outer perimeter of the circuit, gives

\[\begin{equation*}
\tilde{ V}_{d} = \tilde{ V}_{L}+\tilde{ V}_R .
\end{equation*}\]

Straightforward algebra now results in

\[\begin{equation*}
\tilde{ V}_{R} = \frac{\tilde{ V}_{d}}{1+ Z_L/ Z_{C}+ Z_{L}/ Z_R} .
\end{equation*}\]

At high frequencies, the \(Z_{L}/ Z_C\) term, which varies as \(\omega^2\), dominates, so \(\tilde{ V}_R\) and \(\tilde{ I}_R\) are proportional to \(\omega^{-2}\), and the power is proportional to \(\omega^{-4}\).

The flea of subsection 10.3.2 had a long and illustrious
scientific career, and we're now going to pick up her story where we left off.
This flea, whose name is Gauss^{9}, has derived the equation \(E_\perp=2\pi k\sigma\) for the
electric field very close to a charged surface with charge density \(\sigma\).
Next we will describe two improvements she is going to make to that equation.

First, she realizes
that the equation is not as useful as it could be, because it only gives the part of
the field *due to the surface*. If other charges are nearby, then their fields
will add to this field as vectors, and the equation will not be true unless we carefully
subtract out the field from the other charges. This is especially problematic for her
because the planet on which she lives, known for obscure reasons as planet Flatcat, is
itself electrically charged, and so are all the fleas
--- the only thing that keeps them from floating off into
outer space is that they are negatively charged, while Flatcat carries a positive charge, so they
are electrically attracted to it. When Gauss found the original version of her equation,
she wanted to demonstrate it to her skeptical colleagues in the laboratory, using electric
field meters and charged pieces of metal foil. Even if she set up the measurements by
remote control, so that her the charge on her own body would be too far away to have any
effect, they would be disrupted by the ambient field of planet Flatcat. Finally, however,
she realized that she could improve her equation by rewriting it as follows:

\[\begin{equation*}
E_{outward,\ on\ side\ 1}+E_{outward,\ on\ side\ 2} = 4\pi k\sigma .
\end{equation*}\]

The tricky thing here is that “outward” means a different thing, depending on which
side of the foil we're on. On the left side, “outward” means to the left, while on
the right side, “outward” is right. A positively charged piece of metal foil has
a field that points leftward on the left side, and rightward on its right side, so
the two contributions of \(2\pi k\sigma\) are both positive, and we get \(4\pi k\sigma\).
On the other hand, suppose there is a field created by other charges, not by the charged foil,
that happens to point to the right. On the right side, this externally created field is in the same
direction as the foil's field, but on the left side, the it *reduces* the strength
of the leftward field created by the foil. The increase in one term of the equation
balances the decrease in the other term. This new version of the equation is thus
exactly correct regardless of what externally generated fields are present!

Her next innovation starts by multiplying the equation on both sides by the area, \(A\), of one side of the foil:

\[\begin{align*}
\left(E_{outward,\ on\ side\ 1}+E_{outward,\ on\ side\ 2}\right)A &= 4\pi k\sigma A \\
\text{or}
E_{outward,\ on\ side\ 1}A+E_{outward,\ on\ side\ 2}A &= 4\pi kq , \\
\end{align*}\]

where \(q\) is the charge of the foil. The reason for this modification is that
she can now make the whole thing more attractive by
defining a new vector, the area vector **A**. As shown in figure
a, she defines an area vector
for side 1 which has magnitude \(A\) and points outward from side 1, and
an area vector for side 2 which has the same magnitude and points outward from
that side, which is in the opposite direction. The dot product of two vectors,
\(\mathbf{u}\cdot\mathbf{v}\), can be interpreted as \(u_{parallel\ to\ v}|\mathbf{v}|\), and she
can therefore rewrite her equation as

\[\begin{equation*}
\mathbf{E}_1\cdot\mathbf{A}_1+\mathbf{E}_2\cdot\mathbf{A}_2 = 4\pi k q .
\end{equation*}\]

The quantity on the left side of this equation is called the *flux* through
the surface, written \(\Phi\).

Gauss now writes a grant proposal to her favorite funding agency, the BSGS (Blood-Suckers' Geological Survey), and it is quickly approved. Her audacious plan is to send out exploring teams to chart the electric fields of the whole planet of Flatcat, and thereby determine the total electric charge of the planet. The fleas' world is commonly assumed to be a flat disk, and its size is known to be finite, since the sun passes behind it at sunset and comes back around on the other side at dawn. The most daring part of the plan is that it requires surveying not just the known side of the planet but the uncharted Far Side as well. No flea has ever actually gone around the edge and returned to tell the tale, but Gauss assures them that they won't fall off --- their negatively charged bodies will be attracted to the disk no matter which side they are on.

Of course it is possible that the electric charge of planet Flatcat is not perfectly
uniform, but that isn't a problem. As discussed in subsection 10.3.2,
as long as one is very close to the surface, the field only depends on the *local*
charge density. In fact, a side-benefit of Gauss's program of exploration is that any
such local irregularities will be mapped out. But what the newspapers find exciting is
the idea that once all the teams get back from their voyages and tabulate their data,
the *total* charge of the planet will have been determined for the first time.
Each surveying team is assigned to visit a certain list of republics, duchies, city-states, and
so on. They are to record each territory's electric field vector, as well as its area.
Because the electric field may be nonuniform, the final equation for determining the
planet's electric charge will have many terms, not just one for each side of the planet:

\[\begin{equation*}
\Phi = \sum \mathbf{E}_j\cdot\mathbf{A}_j = 4\pi k q_{total}
\end{equation*}\]

Gauss herself leads one of the expeditions, which heads due east, toward the distant Tail Kingdom, known only from fables and the occasional account from a caravan of traders. A strange thing happens, however. Gauss embarks from her college town in the wetlands of the Tongue Republic, travels straight east, passes right through the Tail Kingdom, and one day finds herself right back at home, all without ever seeing the edge of the world! What can have happened? All at once she realizes that the world isn't flat.

Now what? The surveying teams all return, the data are tabulated, and the result for the total charge of Flatcat is \((1/4\pi k)\sum \mathbf{E}_j\cdot\mathbf{A}_j=37\ \text{nC}\) (units of nanocoulombs). But the equation was derived under the assumption that Flatcat was a disk. If Flatcat is really round, then the result may be completely wrong. Gauss and two of her grad students go to their favorite bar, and decide to keep on ordering Bloody Marys until they either solve their problems or forget them. One student suggests that perhaps Flatcat really is a disk, but the edges are rounded. Maybe the surveying teams really did flip over the edge at some point, but just didn't realize it. Under this assumption, the original equation will be approximately valid, and 37 nC really is the total charge of Flatcat.

A second student, named Newton, suggests that they take seriously the possibility that Flatcat is a sphere. In this scenario, their planet's surface is really curved, but the surveying teams just didn't notice the curvature, since they were close to the surface, and the surface was so big compared to them. They divided up the surface into a patchwork, and each patch was fairly small compared to the whole planet, so each patch was nearly flat. Since the patch is nearly flat, it makes sense to define an area vector that is perpendicular to it. In general, this is how we define the direction of an area vector, as shown in figure d. This only works if the areas are small. For instance, there would be no way to define an area vector for an entire sphere, since “outward” is in more than one direction.

If Flatcat is a sphere, then the inside of the sphere must be vast, and there is no way of knowing exactly how the charge is arranged below the surface. However, the survey teams all found that the electric field was approximately perpendicular to the surface everywhere, and that its strength didn't change very much from one location to another. The simplest explanation is that the charge is all concentrated in one small lump at the center of the sphere. They have no way of knowing if this is really the case, but it's a hypothesis that allows them to see how much their 37 nC result would change if they assumed a different geometry. Making this assumption, Newton performs the following simple computation on a napkin. The field at the surface is related to the charge at the center by

\[\begin{equation*}
|\mathbf{E}| &= \frac{kq_{total}}{r^2} ,
\end{equation*}\]

where \(r\) is the radius of Flatcat. The flux is then

\[\begin{equation*}
\Phi &= \sum \mathbf{E}_j\cdot\mathbf{A}_j , \
\end{equation*}\]

and since the \(\mathbf{E}_j\) and \(\mathbf{A}_j\) vectors are parallel, the dot product equals \(|\mathbf{E}_j||\mathbf{A}_j|\), so

\[\begin{equation*}
\Phi &= \sum \frac{kq_{total}}{r^2}|\mathbf{A}_j| .\
\end{equation*}\]

But the field strength is always the same, so we can take it outside the sum, giving

\[\begin{align*}
\Phi &= \frac{kq_{total}}{r^2} \sum |\mathbf{A}_j| \
&= \frac{kq_{total}}{r^2} A_{total} \
&= \frac{kq_{total}}{r^2} 4\pi r^2 \
&= 4\pi kq_{total} .
\end{align*}\]

Not only have all the factors of \(r\) canceled out, but the result is the same as for a disk!

Everyone is pleasantly surprised by this apparent mathematical coincidence, but
is it anything more than that? For instance, what if the charge wasn't concentrated
at the center, but instead was evenly distributed throughout Flatcat's interior
volume? Newton, however, is familiar with a result called the shell theorem
(page 102), which states that the field of a uniformly
charged sphere is the same as if all the charge had been concentrated at its
center.^{10} We now have three different assumptions about the shape of Flatcat and
the arrangement of the charges inside it, and all three lead to exactly the
*same* mathematical result, \(\Phi = 4\pi kq_{total}\). This is starting to
look like more than a coincidence. In fact, there is a general mathematical theorem,
called Gauss' theorem, which states the following:

For any region of space, the flux through the surface equals \(4\pi kq_{in}\), where \(q_{in}\) is the total charge in that region.

Don't memorize the factor of \(4\pi\) in front --- you can rederive it any time you need to, by considering a spherical surface centered on a point charge.

Note that although region and its surface had a definite physical existence in our story --- they are the planet Flatcat and the surface of planet Flatcat --- Gauss' law is true for any region and surface we choose, and in general, the Gaussian surface has no direct physical significance. It's simply a computational tool.

Rather than proving Gauss' theorem and then presenting some examples and applications, it turns out to be easier to show some examples that demonstrate its salient properties. Having understood these properties, the proof becomes quite simple.

Suppose we have a negative point charge, whose field points inward, and we pick a Gaussian surface which is a sphere centered on that charge. How does Gauss' theorem apply here?

(answer in the back of the PDF version of the book)Figure e shows two two different ways in which flux is additive. Figure e/1, additivity by charge, shows that we can break down a charge distribution into two or more parts, and the flux equals the sum of the fluxes due to the individual charges. This follows directly from the fact that the flux is defined in terms of a dot product, \(\mathbf{E}\cdot\mathbf{A}\), and the dot product has the additive property \((\mathbf{a}+\mathbf{b})\cdot\mathbf{c}=\mathbf{a}\cdot\mathbf{c}+\mathbf{b}\cdot\mathbf{c}\).

To understand additivity of flux by region, e/2, we have to consider the parts of the two surfaces that were eliminated when they were joined together, like knocking out a wall to make two small apartments into one big one. Although the two regions shared this wall before it was removed, the area vectors were opposite: the direction that is outward from one region is inward with respect to the other. Thus if the field on the wall contributes positive flux to one region, it contributes an equal amount of negative flux to the other region, and we can therefore eliminate the wall to join the two regions, without changing the total flux.

A third important property of Gauss' theorem is that it only refers to the charge
*inside* the region we choose to discuss. In other words, it asserts that any
charge outside the region contributes zero to the flux. This makes at least some sense, because
a charge outside the region will have field vectors pointing into the surface on one
side, and out of the surface on the other. Certainly there
should be at least partial cancellation between the
negative (inward) flux on one side and the positive (outward) flux on the other. But why
should this cancellation be exact?

To see the reason for this perfect cancellation, we can imagine space as being built out of tiny cubes, and we can think of any charge distribution as being composed of point charges. The additivity-by-charge property tells us that any charge distribution can be handled by considering its point charges individually, and the additivity-by-region property tells us that if we have a single point charge outside a big region, we can break the region down into tiny cubes. If we can prove that the flux through such a tiny cube really does cancel exactly, then the same must be true for any region, which we could build out of such cubes, and any charge distribution, which we can build out of point charges.

For simplicity, we will carry out this calculation only in the special case shown in figure f, where the charge lies along one axis of the cube. Let the sides of the cube have length \(2b\), so that the area of each side is \((2b)^2=4b^2\). The cube extends a distance \(b\) above, below, in front of, and behind the horizontal \(x\) axis. There is a distance \(d-b\) from the charge to the left side, and \(d+b\) to the right side.

There will be one negative flux, through the left side, and five positive ones. Of these positive ones, the one through the right side is very nearly the same in magnitude as the negative flux through the left side, but just a little less because the field is weaker on the right, due to the greater distance from the charge. The fluxes through the other four sides are very small, since the field is nearly perpendicular to their area vectors, and the dot product \(\mathbf{E}_j\cdot\mathbf{A}_j\) is zero if the two vectors are perpendicular. In the limit where \(b\) is very small, we can approximate the flux by evaluating the field at the center of each of the cube's six sides, giving

\[\begin{align*}
\Phi &= \Phi_{left}+4\Phi_{side}+\Phi_{right} \\
&= |\mathbf{E}_{left}||\mathbf{A}_{left}|\cos 180°
+4|\mathbf{E}_{side}||\mathbf{A}_{side}|\cos \theta_{side} \\
& +|\mathbf{E}_{right}||\mathbf{A}_{right}|\cos 0° ,\\
\text{and a little trig gives $\cos\theta_{side}\approx b/d$, so}
\Phi &= -|\mathbf{E}_{left}||\mathbf{A}_{left}|
+4|\mathbf{E}_{side}||\mathbf{A}_{side}|\frac{b}{d}
+|\mathbf{E}_{right}||\mathbf{A}_{right}|\\
&= \left(4b^2\right)\left(-|\mathbf{E}_{left}|
+4|\mathbf{E}_{side}|\frac{b}{d}
+|\mathbf{E}_{right}|\right)\\
&= \left(4b^2\right)\left(-\frac{kq}{(d-b)^2}
+4\frac{kq}{d^2}\frac{b}{d}
+\frac{kq}{(d+b)^2}\right)\\
&= \left(\frac{4kqb^2}{d^2}\right)\left(-\frac{1}{(1-b/d)^2}
+\frac{4b}{d}
+\frac{1}{(1+b/d)^2}\right) .\\
\text{Using the approximation $(1+\epsilon)^{-2}\approx 1-2\epsilon$ for small $\epsilon$, this
becomes}
\Phi &= \left(\frac{4kqb^2}{d^2}\right)\left(-1-\frac{2b}{d}
+\frac{4b}{d}
+1-\frac{2b}{d}\right) \\
&= 0 .
\end{align*}\]

Thus in the limit of a very small cube, \(b\ll d\), we have proved that the flux due to
this exterior charge is zero. The proof can be extended to the case where the
charge is not along any axis of the
cube,^{11}
and based on additivity we then have a proof that the flux due to an outside charge is
always zero.

◊

One question that might naturally occur to you about Gauss's law is what happens for charge that is exactly on the surface --- should it be counted toward the enclosed charge, or not? If charges can be perfect, infinitesimal points, then this could be a physically meaningful question. Suppose we approach this question by way of a limit: start with charge \(q\) spread out over a sphere of finite size, and then make the size of the sphere approach zero. The figure shows a uniformly charged sphere that's exactly half-way in and half-way out of the cubical Gaussian surface. What is the flux through the cube, compared to what it would be if the charge was entirely enclosed? (There are at least three ways to find this flux: by direct integration, by Gauss's law, or by the additivity of flux by region.)

◊

The dipole is completely enclosed in the cube. What does Gauss's law say about the flux through the cube? If you imagine the dipole's field pattern, can you verify that this makes sense?

◊

The wire passes in through one side of the cube and out through the other. If the current through the wire is increasing, then the wire will act like an inductor, and there will be a voltage difference between its ends. (The inductance will be relatively small, since the wire isn't coiled up, and the \(\Delta V\) will therefore also be fairly small, but still not zero.) The \(\Delta V\) implies the existence of electric fields, and yet Gauss's law says the flux must be zero, since there is no charge inside the cube. Why isn't Gauss's law violated?

◊

The charge has been loitering near the edge of the cube, but is then suddenly hit with a mallet, causing it to fly off toward the left side of the cube. We haven't yet discussed in detail how disturbances in the electric and magnetic fields ripple outward through space, but it turns out that they do so at the speed of light. (In fact, that's what light is: ripples in the electric and magnetic fields.) Because the charge is closer to the left side of the cube, the change in the electric field occurs there before the information reaches the right side. This would seem certain to lead to a violation of Gauss's law. How can the ideas explored in discussion question C show the resolution to this paradox?

With the computational machinery we've developed, it is now simple to prove Gauss' theorem. Based on additivity by charge, it suffices to prove the law for a point charge. We have already proved Gauss' law for a point charge in the case where the point charge is outside the region. If we can prove it for the inside case, then we're all done.

If the charge is inside, we reason as follows. First, we forget about the actual Gaussian surface of interest, and instead construct a spherical one, centered on the charge. For the case of a sphere, we've already seen the proof written on a napkin by the flea named Newton (page 621). Now wherever the actual surface sticks out beyond the sphere, we glue appropriately shaped pieces onto the sphere. In the example shown in figure h, we have to add two Mickey Mouse ears. Since these added pieces do not contain the point charge, the flux through them is zero, and additivity of flux by region therefore tells us that the total flux is not changed when we make this alteration. Likewise, we need to chisel out any regions where the sphere sticks out beyond the actual surface. Again, there is no change in flux, since the region being altered doesn't contain the point charge. This proves that the flux through the Gaussian surface of interest is the same as the flux through the sphere, and since we've already proved that that flux equals \(4\pi kq_{in}\), our proof of Gauss' theorem is complete.

◊

A critical part of the proof of Gauss' theorem was the proof that a tiny cube has zero flux through it due to an external charge. Discuss qualitatively why this proof would fail if Coulomb's law was a \(1/r\) or \(1/r^3\) law.

Note that the proof of Gauss' theorem depended on the computation on the napkin
discussed on page 10.6.1. The crucial point in this computation was that
the electric field of a point charge falls off like \(1/r^2\), and since the
area of a sphere is proportional to \(r^2\), the result is independent of \(r\).
The \(1/r^2\) variation of the field also came into play on page 624
in the proof that the flux due to an outside charge is zero.
In other words, if we discover some other force of nature which is proportional to
\(1/r^3\) or \(r\), then Gauss' theorem will not apply to that force. Gauss' theorem
is not true for nuclear forces, which fall off exponentially with distance. However, this
is the *only* assumption we had to make about the nature of the field. Since
gravity, for instance, also has fields that fall off as \(1/r^2\), Gauss' theorem
is equally valid for gravity --- we just have to replace mass with
charge, change the Coulomb constant \(k\) to the gravitational constant
\(G\), and insert a minus sign because the gravitational fields around a (positive)
mass point inward.

Gauss' theorem can only be proved if we assume a \(1/r^2\) field, and the converse
is also true: any field that satisfies Gauss' theorem must be a \(1/r^2\) field.
Thus although we previously thought of Coulomb's law as the fundamental law
of nature describing electric forces, it is equally valid to think of Gauss'
theorem as the basic law of nature for electricity. From this point of view,
Gauss' theorem is not a mathematical fact but an experimentally testable statement
about nature, so we'll refer to it as Gauss' *law*, just as we speak of
Coulomb's *law* or Newton's *law* of gravity.

If Gauss' law is equivalent to Coulomb's law, why not just use Coulomb's law? First, there are some cases where calculating a field is easy with Gauss' law, and hard with Coulomb's law. More importantly, Gauss' law and Coulomb's law are only mathematically equivalent under the assumption that all our charges are standing still, and all our fields are constant over time, i.e., in the study of electrostatics, as opposed to electrodynamics. As we broaden our scope to study generators, inductors, transformers, and radio antennas, we will encounter cases where Gauss' law is valid, but Coulomb's law is not.

Often we encounter situations where we have a static charge distribution, and we wish to determine the field. Although superposition is a generic strategy for solving this type of problem, if the charge distribution is symmetric in some way, then Gauss' law is often a far easier way to carry out the computation.

Consider the field of an infinitely long line of charge, holding a uniform charge per unit length \(\lambda\). Computing this field by brute-force superposition was fairly laborious (examples 10 on page 576 and 13 on page 582). With Gauss' law it becomes a very simple calculation.

The problem has two types of symmetry. The line of charge, and therefore the resulting field pattern, look the same if we rotate them about the line. The second symmetry occurs because the line is infinite: if we slide the line along its own length, nothing changes. This sliding symmetry, known as a translation symmetry, tells us that the field must point directly away from the line at any given point.

Based on these symmetries, we choose the Gaussian surface shown in figure i. If we want to know the field at a distance \(R\) from the line, then we choose this surface to have a radius \(R\), as shown in the figure. The length, \(L\), of the surface is irrelevant.

The field is parallel to the surface on the end caps, and therefore perpendicular to the end caps' area vectors, so there is no contribution to the flux. On the long, thin strips that make up the rest of the surface, the field is perpendicular to the surface, and therefore parallel to the area vector of each strip, so that the dot product occurring in the definition of the flux is \(\mathbf{E}_j\cdot\mathbf{A}_j=|\mathbf{E}_j||\mathbf{A}_j||\cos\ 0°=|\mathbf{E}_j||\mathbf{A}_j|\). Gauss' law gives

\[\begin{align*}
4\pi k q_{in} &= \sum \mathbf{E}_j\cdot\mathbf{A}_j \\
4\pi k \lambda L &= \sum |\mathbf{E}_j||\mathbf{A}_j| .\\
\text{The magnitude of the field is the same on every strip, so we can take it outside the sum.}
4\pi k \lambda L &= |\mathbf{E}| \sum |\mathbf{A}_j| \\
\text{In the limit where the strips are infinitely narrow, the surface becomes a
cylinder, with (area)=(circumference)(length)=$2\pi RL$.}
4\pi k \lambda L &= |\mathbf{E}| \times 2\pi RL \\
|\mathbf{E}| &= \frac{2k\lambda}{R} \\
\end{align*}\]

As claimed earlier, the result \(E=2\pi k\sigma\) for the field near a charged surface is a special case of Gauss' law. We choose a Gaussian surface of the shape shown in figure j, known as a Gaussian pillbox. The exact shape of the flat end caps is unimportant.

The symmetry of the charge distribution tells us that the field points directly away from the surface, and is equally strong on both sides of the surface. This means that the end caps contribute equally to the flux, and the curved sides have zero flux through them. If the area of each end cap is \(A\), then

\[\begin{align*}
4\pi k q_{in} &= \mathbf{E}_1\cdot\mathbf{A}_1+\mathbf{E}_2\cdot\mathbf{A}_2 , \\
\text{where the subscripts 1 and 2 refer to the two end caps. We have $\mathbf{A}_2=-\mathbf{A}_1$, so}
4\pi k q_{in} &= \mathbf{E}_1\cdot\mathbf{A}_1-\mathbf{E}_2\cdot\mathbf{A}_1 \\
4\pi k q_{in} &= \left(\mathbf{E}_1-\mathbf{E}_2\right)\cdot\mathbf{A}_1 , \\
\text{and by symmetry the magnitudes of the two fields are equal, so}
2|\mathbf{E}|A &= 4 \pi k \sigma A\\
|\mathbf{E}| &= 2\pi k\sigma
\end{align*}\]

The symmetry between the two sides could be broken by the existence of other charges nearby, whose fields would add onto the field of the surface itself. Even then, Gauss's law still guarantees

\[\begin{align*}
4\pi k q_{in} &= \left(\mathbf{E}_1-\mathbf{E}_2\right)\cdot\mathbf{A}_1 ,
\text{or}
|\mathbf{E}_{\perp,1}-\mathbf{E}_{\perp,2}| &= 4\pi k \sigma ,
\end{align*}\]

where the subscript \(\perp\) indicates the component of the field parallel to the surface (i.e., parallel to the area vectors). In other words, the electric field changes discontinuously when we pass through a charged surface; the discontinuity occurs in the component of the field perpendicular to the surface, and the amount of discontinuous change is \(4\pi k \sigma\). This is a completely general statement that is true near any charged surface, regardless of the existence of other charges nearby.

Gauss' law is a bit spooky. It relates the field on the Gaussian surface to the charges inside the surface. What if the charges have been moving around, and the field at the surface right now is the one that was created by the charges in their previous locations? Gauss' law --- unlike Coulomb's law --- still works in cases like these, but it's far from obvious how the flux and the charges can still stay in agreement if the charges have been moving around.

For this reason, it would be more physically attractive to restate Gauss'
law in a different form, so that it related the behavior of the field
at one point to the charges that were actually present at that point.
This is essentially what we were doing in the fable of the flea named
Gauss: the fleas' plan for surveying their planet was essentially one of
dividing up the surface of their planet (which they believed was flat)
into a patchwork, and then constructing *small* a Gaussian pillbox
around each *small* patch. The equation \(E_{\perp}=2\pi k\sigma\)
then related a particular property of the *local* electric field to
the *local* charge density.

In general, charge distributions need not be confined to a flat surface --- life is three-dimensional --- but the general approach of defining very small Gaussian surfaces is still a good one. Our strategy is to divide up space into tiny cubes, like the one on page 623. Each such cube constitutes a Gaussian surface, which may contain some charge. Again we approximate the field using its six values at the center of each of the six sides. Let the cube extend from \(x\) to \(x+dx\), from \(y\) to \(y+dy\), and from \(y\) to \(y+dy\).

The sides at \(x\) and \(x+dx\) have area vectors \(-dydz\hat{\mathbf{x}}\) and \(dydz\hat{\mathbf{x}}\), respectively. The flux through the side at \(x\) is \(-E_x(x)dydz\), and the flux through the opposite side, at \(x+dx\) is \(E_x(x+dx)dydz\). The sum of these is \((E_x(x+dx)-E_x(x))dydz\), and if the field was uniform, the flux through these two opposite sides would be zero. It will only be zero if the field's \(x\) component changes as a function of \(x\). The difference \(E_x(x+dx)-E_x(x)\) can be rewritten as \(dE_x=(dE_x)/(dx)dx\), so the contribution to the flux from these two sides of the cube ends up being

\[\begin{equation*}
\frac{dE_x}{dx}dxdydz .
\end{equation*}\]

Doing the same for the other sides, we end up with a total flux

\[\begin{align*}
d \Phi &= \left(\frac{dE_x}{dx}+\frac{dE_y}{dy}
+\frac{dE_z}{dz}\right)dxdydz \\
&= \left(\frac{dE_x}{dx}+\frac{dE_y}{dy}
+\frac{dE_z}{dz}\right)dv ,\\
\text{where $dv$ is the volume of the cube. In evaluating each of these
three derivatives, we are going to treat the other two variables as constants,
to emphasize this we use the partial derivative notation $\partial$ introduced
in chapter 3,}
d \Phi &= \left(\frac{\partial E_x}{\partial x}+\frac{\partial E_y}{\partial y}
+\frac{\partial E_z}{\partial z}\right)dv .\\
\text{Using Gauss' law,}
4\pi k q_{in} &= \left(\frac{\partial E_x}{\partial x}+\frac{\partial E_y}{\partial y}
+\frac{\partial E_z}{\partial z}\right)dv ,\\
\text{and we introduce the notation $\rho$ (Greek letter rho) for the charge
per unit volume, giving}
4\pi k \rho &= \frac{\partial E_x}{\partial x}+\frac{\partial E_y}{\partial y}
+\frac{\partial E_z}{\partial z} .\\
\text{The quantity on the right is called the *divergence* of the electric
field, written $\divg \mathbf{E}$. Using this notation, we have}
\divg \mathbf{E} = 4\pi k \rho .
\end{align*}\]

This equation has all the same physical implications as Gauss' law. After all, we proved Gauss' law by breaking down space into little cubes like this. We therefore refer to it as the differential form of Gauss' law, as opposed to \(\Phi=4\pi kq_{in}\), which is called the integral form.

Figure b shows an intuitive way of visualizing the meaning of the divergence. The meter consists of some electrically charged balls connected by springs. If the divergence is positive, then the whole cluster will expand, and it will contract its volume if it is placed at a point where the field has \(\divg\mathbf{E}\lt0\). What if the field is constant? We know based on the definition of the divergence that we should have \(\divg\mathbf{E}=0\) in this case, and the meter does give the right result: all the balls will feel a force in the same direction, but they will neither expand nor contract.

\(\triangleright\) Intuitively, we can see that no matter where we put the div-meter in this field, it will neither expand nor contract. For instance, if we put it at the center of the figure, it will start spinning, but that's it.

Mathematically, let the \(x\) axis be to the right and let \(y\) be up. The field is of the form

\[\begin{equation*}
\mathbf{E} = (\text{sin} Kx)\: \hat{\mathbf{y}} ,
\end{equation*}\]

where the constant \(K\) is not to be confused with Coulomb's constant. Since the field has only a \(y\) component, the only term in the divergence we need to evaluate is

\[\begin{equation*}
\mathbf{E} = \frac{\partial E_{y}}{\partial y} ,
\end{equation*}\]

but this vanishes, because \(E_y\) depends only on \(x\), not \(y\) : we treat \(y\) as a constant when evaluating the partial derivative \(\partial E_{y}/\partial y\), and the derivative of an expression containing only constants must be zero.

Physically this is a very important result: it tells us that a light wave can exist without any charges along the way to “keep it going.” In other words, light can travel through a vacuum, a region with no particles in it. If this wasn't true, we'd be dead, because the sun's light wouldn't be able to get to us through millions of kilometers of empty space!

At all other points, we have

\[\begin{equation*}
\mathbf{E} = \frac{ kq}{ r^2}\hat{\mathbf{r}} ,
\end{equation*}\]

where \(\hat{\mathbf{r}}=\mathbf{r}/ r=( x\hat{\mathbf{x}}+ y\hat{\mathbf{y}}+ z\hat{\mathbf{z}})/ r\) is the unit vector pointing radially away from the charge. The field can therefore be written as

\[\begin{align*}
\mathbf{E} &= \frac{ kq}{ r^3}\hat{\mathbf{r}} \\
&= \frac{ kq( x\hat{\mathbf{x}}+ y\hat{\mathbf{y}}+ z\hat{\mathbf{z}})}{\left( x^2+ y^2+ z^2\right)^\text{3/2}} . \\
\text{The three terms in the divergence are all similar, e.g.,}
\frac{\partial E_{x}}{\partial x}
&= kq\frac{\partial}{\partial x}\left[\frac{ x}{\left( x^2+ y^2+ z^2\right)^\text{3/2}}\right] \\
&= kq\left[\frac{1}{\left( x^2+ y^2+ z^2\right)^\text{3/2}}-\frac{3}{2}\:\frac{2 x^2}{\left( x^2+ y^2+ z^2\right)^\text{5/2}}\right] \\
&= kq\left( r^{-3}-3 x^2 r^{-5}\right) .
\end{align*}\]

Straightforward algebra shows that adding in the other two terms results in zero, which makes sense, because there is no charge except at the origin.

Gauss' law in differential form lends itself most easily to finding the charge density when we are give the field. What if we want to find the field given the charge density? As demonstrated in the following example, one technique that often works is to guess the general form of the field based on experience or physical intuition, and then try to use Gauss' law to find what specific version of that general form will be a solution.

\(\triangleright\) By symmetry we know that the field must be purely radial (in and out). We guess that the solution might be of the form

\[\begin{equation*}
\mathbf{E} = br^ p\hat{\mathbf{r}} ,
\end{equation*}\]

where \(r\) is the distance from the center, and \(b\) and \(p\) are constants. A negative value of \(p\) would indicate a field that was strongest at the center, while a positive \(p\) would give zero field at the center and stronger fields farther out. Physically, we know by symmetry that the field is zero at the center, so we expect \(p\) to be positive.

As in the example 37, we rewrite \(\hat{\mathbf{r}}\) as \(\mathbf{r}/ r\), and to simplify the writing we define \(n= p-1\), so

\[\begin{equation*}
\mathbf{E} = br^ n\mathbf{r} .
\end{equation*}\]

Gauss' law in differential form is

\[\begin{equation*}
\divg\mathbf{E} = 4\pi k\rho ,
\end{equation*}\]

so we want a field whose divergence is constant. For a field of the form we guessed, the divergence has terms in it like

\[\begin{align*}
\frac{\partial E_{x}}{\partial x}
&= \frac{\partial}{\partial x}\left( br^{n} x\right) \\
&= b\left( nr^{ n-1}\frac{\partial r}{\partial x} x+r^ n\right) \\
\end{align*}\]

The partial derivative \(\partial r/\partial x\) is easily calculated to be \(x/ r\), so

\[\begin{equation*}
\frac{\partial E_{x}}{\partial x}
= b\left( nr^{ n-2} x^2+r^ n\right)
\end{equation*}\]

Adding in similar expressions for the other two terms in the divergence, and making use of \(x^2+ y^2+ z^2= r^2\), we have

\[\begin{equation*}
\divg\mathbf{E} = b( n+3) r^ n .
\end{equation*}\]

This can indeed be constant, but only if \(n\) is 0 or \(-3\),
i.e., \(p\) is 1 or \(-2\).
The second solution gives a divergence which is constant and *zero* :
this is the solution for the *outside* of the sphere! The first
solution, which has the field directly proportional to \(r\),
must be the one that applies to the inside of the sphere,
which is what we care about right now.
Equating the
coefficient in front to the one in Gauss' law, the field is

\[\begin{equation*}
\mathbf{E} = \frac{4\pi k\rho}{3} r\:\hat{\mathbf{r}} .
\end{equation*}\]

The field is zero at the center, and gets stronger and stronger as we approach the surface.

◊

As suggested by the figure, discuss the results you would get by inserting the div-meter at various locations in the sine-wave field.

\backofchapterboilerplate{efield}

\begin{homeworkforcelabel}{sparkplug}{0}{}{1}The gap between the electrodes in an automobile
engine's spark plug is 0.060 cm. To produce an electric
spark in a gasoline-air mixture, an electric field of
\(3.0\times10^6\) V/m must be achieved. On starting a car,
what minimum voltage must be supplied by the ignition
circuit? Assume the field is uniform.(answer check available at lightandmatter.com)

(b) The small size
of the gap between the electrodes is inconvenient because it
can get blocked easily, and special tools are needed to
measure it. Why don't they design spark plugs with a wider gap?
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{distantrsquared}{1}{}{2}(a) As suggested in example 9 on page 575,
use approximations to show that the expression given for the
electric field approaches \(kQ/d^2\) for large \(d\).

(b) Do the same for the result of example 12
on page 579.
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{galaxy-mass}{1}{}{3}Astronomers believe that the mass distribution (mass per unit volume) of some galaxies may be approximated, in spherical coordinates, by \(\rho=ae^{-br}\), for \(0\le r\le\infty\), where \(\rho\) is the density. Find the total mass. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{chargemotioninfield}{0}{}{4}(a) At time \(t=0\), a positively charged particle is
placed, at rest, in a vacuum, in which there is
a uniform electric field of magnitude
\(E\). Write an equation giving the particle's speed, \(v\), in terms of
\(t\), \(E\), and its mass and charge \(m\) and \(q\).(answer check available at lightandmatter.com)

(b) If this is done with two different objects and they are
observed to have the same motion, what can you conclude
about their masses and charges? (For instance, when
radioactivity was discovered, it was found that one form of
it had the same motion as an electron in this type of experiment.)
\end{homeworkforcelabel}
\begin{homeworkforcelabel}{altedefunits}{0}{}{5}Show that the alternative definition of the magnitude of the electric field,
\(|**E**|=\tau/D_t\sin\theta\), has units that make sense.
\end{homeworkforcelabel}
\begin{homeworkforcelabel}{dipole-change-origin}{1}{}{6}Redo the calculation of example 5 on page
568 using a different origin for the coordinate system,
and show that you get the same result.
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{dipolechoiceoforigin}{1}{}{7}The definition of the dipole moment, \(\mathbf{D}=\sum q_i \mathbf{r}_i\),
involves the vector \(\mathbf{r}_i\) stretching from the origin of our coordinate
system out to the charge \(q_i\). There are clearly cases where this
causes the dipole moment to be dependent on the choice of coordinate
system. For instance, if there is only one charge, then we could make
the dipole moment equal zero if we chose the origin to be right on top
of the charge, or nonzero if we put the origin somewhere else.

(a) Make up a numerical example with two charges of equal magnitude
and opposite sign. Compute the dipole moment using two different coordinate
systems that are oriented the same way, but differ in the choice of origin.
Comment on the result.

(b) Generalize the result of part a to any pair of charges with equal
magnitude and opposite sign. This is supposed to be a proof for *any*
arrangement of the two charges, so don't assume any numbers.

(c) Generalize further, to \(n\) charges.
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{lineandsquaredipoles}{1}{}{8}Compare the two dipole moments. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{quadrupole}{1}{}{9}Find an arrangement of charges that has zero total charge and zero dipole moment, but that will make nonvanishing electric fields. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{ringve}{0}{}{10}As suggested in example 11 on page 577, show that you can get the same result for the on-axis field by differentiating the voltage \end{homeworkforcelabel}

\begin{homeworkforcelabel}{esquare}{1}{}{11}Three charges are arranged on a square as shown. All three charges are positive. What value of \(q_2/q_1\) will produce zero electric field at the center of the square?(answer check available at lightandmatter.com) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{dipolefarfield}{0}{}{12}This is a one-dimensional problem, with everything confined to
the \(x\) axis. Dipole A consists of a \(-1.000\) C charge at \(x=0.000\) m
and a \(1.000\) C charge at \(x=1.000\) m. Dipole B has
a \(-2.000\) C charge at \(x=0.000\) m
and a \(2.000\) C charge at \(x=0.500\) m.

(a) Compare the two dipole moments.

(b) Calculate the field created by dipole A at \(x=10.000\) m,
and compare with the field dipole B would make. Comment on the
result.(answer check available at lightandmatter.com)
\end{homeworkforcelabel}
\begin{homeworkforcelabel}{neuronfield}{1}{}{13}In our by-now-familiar neuron, the voltage difference
between the inner and outer surfaces of the cell membrane is
about \(V_{out}-V_{in}=-70\ \text{mV}\) in the resting state, and the
thickness of the membrane is about 6.0 nm (i.e., only about a
hundred atoms thick). What is the electric field inside the membrane?(answer check available at lightandmatter.com)
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{proton-in-nonuniform-field}{1}{}{14}A proton is in a region in which the electric field is given by \(E=a+bx^3\). If the proton starts at rest at \(x_1=0\), find its speed, \(v\), when it reaches position \(x_2\). Give your answer in terms of \(a\), \(b\), \(x_2\), and \(e\) and \(m\), the charge and mass of the proton.(answer check available at lightandmatter.com) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{dipolev}{1}{}{15}(a) Given that the on-axis field of a dipole at large distances is proportional to
\(D/r^3\), show that its voltage
varies as \(D/r^2\). (Ignore positive and negative signs and
numerical constants of proportionality.)

(b) Write down an exact expression for the voltage of a two-charge dipole at an on-axis point,
without assuming that the distance is large compared to the size
of the dipole. Your expression will have to contain the actual
charges and size of the dipole, not just its dipole moment. Now
use approximations to show that, at large distances, this is consistent with
your answer to part a.\hwhint{hwhint:dipolev}
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{screened}{1}{}{16}A hydrogen atom is electrically neutral, so at large distances, we expect that it will create essentially zero electric field. This is not true, however, near the atom or inside it. Very close to the proton, for example, the field is very strong. To see this, think of the electron as a spherically symmetric cloud that surrounds the proton, getting thinner and thinner as we get farther away from the proton. (Quantum mechanics tells us that this is a more correct picture than trying to imagine the electron orbiting the proton.) Near the center of the atom, the electron cloud's field cancels out by symmetry, but the proton's field is strong, so the total field is very strong. The voltage in and around the hydrogen atom can be approximated using an expression of the form \(V=r^{-1}e^{-r}\). (The units come out wrong, because I've left out some constants.) Find the electric field corresponding to this voltage, and comment on its behavior at very large and very small \(r\). (solution in the pdf version of the book) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{carbondioxide}{0}{}{17} A carbon dioxide molecule is structured like O-C-O, with all three atoms along a line. The oxygen atoms grab a little bit of extra negative charge, leaving the carbon positive. The molecule's symmetry, however, means that it has no overall dipole moment, unlike a V-shaped water molecule, for instance. Whereas the voltage of a dipole of magnitude \(D\) is proportional to \(D/r^2\) (see problem 15), it turns out that the voltage of a carbon dioxide molecule at a distant point along the molecule's axis equals \(b/r^3\), where \(r\) is the distance from the molecule and \(b\) is a constant (cf. problem 9). What would be the electric field of a carbon dioxide molecule at a point on the molecule's axis, at a distance \(r\) from the molecule?(answer check available at lightandmatter.com) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{electron-cloud}{1}{}{18}A hydrogen atom in a particular state has the charge density (charge per unit volume) of the electron cloud given by \(\rho=ae^{-br}z^2\), where \(r\) is the distance from the proton, and \(z\) is the coordinate measured along the \(z\) axis. Given that the total charge of the electron cloud must be \(-e\), find \(a\) in terms of the other variables. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{dipolemidplane}{2}{}{19}A dipole has a midplane, i.e., the plane that cuts through the dipole's center, and is perpendicular to the dipole's axis. Consider a two-charge dipole made of point charges \(\pm q\) located at \(z=\pm\ell/2\). Use approximations to find the field at a distant point in the midplane, and show that its magnitude comes out to be \(kD/R^3\) (half what it would be at a point on the axis lying an equal distance from the dipole). \end{homeworkforcelabel}

\begin{homeworkforcelabel}{hyperbolic}{0}{}{20}The figure shows a vacuum chamber surrounded by four metal electrodes shaped like hyperbolas. (Yes, physicists do sometimes ask their university machine shops for things machined in mathematical shapes like this. They have to be made on computer-controlled mills.) We assume that the electrodes extend far into and out of the page along the unseen \(z\) axis, so that by symmetry, the electric fields are the same for all \(z\). The problem is therefore effectively two-dimensional. Two of the electrodes are at voltage \(+V_\text{o}\), and the other two at \(-V_\text{o}\), as shown. The equations of the hyperbolic surfaces are \(|xy|=b^2\), where \(b\) is a constant. (We can interpret \(b\) as giving the locations \(x=\pm b\), \(y=\pm b\) of the four points on the surfaces that are closest to the central axis.) There is no obvious, pedestrian way to determine the field or voltage in the central vacuum region, but there's a trick that works: with a little mathematical insight, we see that the voltage \(V=V_\text{o}b^{-2}xy\) is consistent with all the given information. (Mathematicians could prove that this solution was unique, but a physicist knows it on physical grounds: if there were two different solutions, there would be no physical way for the system to decide which one to do!) (a) Use the techniques of subsection 10.2.2 to find the field in the vacuum region, and (b) sketch the field as a “sea of arrows.”(answer check available at lightandmatter.com) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{quadraticvoltage}{1}{}{21}(a) A certain region of three-dimensional space has a voltage that varies as
\(V=br^2\), where \(r\) is the distance from the origin.
Use the techniques of subsection 10.2.2
to find the field.(answer check available at lightandmatter.com)

(b) Write down another voltage that gives exactly the same field.
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{estrips}{1}{}{22}(a) Example 10 on page 576
gives the field of a charged rod in its midplane.
Starting from this result, take the limit as the length of the rod approaches infinity.
Note that \(\lambda\) is not changing, so as \(L\) gets bigger, the total charge \(Q\) increases.
\hwans{hwans:estrips}

(b) In the text, I have shown (by several different methods)
that the field of an infinite,
uniformly charged plane is \(2\pi k\sigma\). Now you're going to
rederive the same result by a different method.
Suppose that it is the \(x-y\) plane that is charged, and we
want to find the field at the point \((0,0,z)\). (Since the plane
is infinite, there is no loss of generality in assuming
\(x=0\) and \(y=0\).)
Imagine that we slice the plane into an infinite number of
straight strips parallel to the \(y\) axis.
Each strip has infinitesimal width \(dx\), and extends
from \(x\) to \(x+dx\). The contribution any one of these
strips to the field at our point has a magnitude which can
be found from part a.
By vector addition, prove the desired result for the field of
the plane of charge.
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{halfinfinitecylinder}{1}{}{23}Consider the electric field created by a uniformly
charged cylindrical surface that extends to infinity in one direction.

(a) Show that the
field at the center of the cylinder's mouth is \(2\pi k\sigma\),
which happens to be the same as the field of an infinite *flat*
sheet of charge!

(b) This expression is independent of the radius of the
cylinder. Explain why this should be so. For example, what
would happen if you doubled the cylinder's radius?
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{lightning}{1}{}{24}
In an electrical storm, the cloud and the ground act like
a parallel-plate capacitor, which typically charges up due
to frictional electricity in collisions of ice particles in
the cold upper atmosphere. Lightning occurs when the
magnitude of the electric field builds up to a critical
value, \(E_c\), at which air is ionized.

(a) Treat the cloud as a flat square with sides of length
\(L\). If it is at a height \(h\) above the ground, find the
amount of energy released in the lightning strike.(answer check available at lightandmatter.com)

(b) Based on your answer from part a, which is more
dangerous, a lightning strike from a high-altitude cloud
or a low-altitude one?

(c) Make an order-of-magnitude estimate of the energy
released by a typical lightning bolt, assuming reasonable
values for its size and altitude. \(E_c\) is about \(10^6\) V/m.
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{epointinfty}{1}{}{25}(a) Show that the energy in the electric field of a point charge
is infinite! Does the integral diverge at small distances, at large
distances, or both? \hwhint{hwhint:epointinfty}

[4]
(b) Now calculate the energy in the electric field of a uniformly
charged sphere with radius \(b\). Based on the shell theorem,
it can be shown that the field for \(r>b\) is the same as for
a point charge, while the field for \(r\ltb\) is \(kqr/b^3\). (Example
38 shows this using a different technique.)

The calculation in part a seems to show that infinite energy
would be required in order to create a charged, pointlike particle.
However, there are processes that, for example,
create electron-positron pairs, and these processes don't require
infinite energy. According to Einstein's famous equation
\(E=mc^2\), the energy required to create such a pair should only
be \(2mc^2\), which is finite. One way out of this difficulty is to
assume that no particle is really pointlike, and this is in fact the
main motivation behind a speculative physical theory called string
theory, which posits that charged particles are actually tiny loops,
not points.

(answer check available at lightandmatter.com) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{neuronenergy}{1}{}{26}
The neuron in the figure has been drawn fairly short, but
some neurons in your spinal cord have tails (axons) up to a
meter long. The inner and outer surfaces of the membrane act
as the “plates” of a capacitor. (The fact that it has been
rolled up into a cylinder has very little effect.) In order
to function, the neuron must create a voltage difference \(V\)
between the inner and outer surfaces of the membrane. Let
the membrane's thickness, radius, and length be \(t\), \(r\), and \(L\).
(a) Calculate the energy that must be stored in the electric
field for the neuron to do its job. (In real life, the
membrane is made out of a substance called a dielectric,
whose electrical properties increase the amount of energy
that must be stored. For the sake of this analysis, ignore
this fact.)
\hwhint{hwhint:neuronenergy}(answer check available at lightandmatter.com)

(b) An organism's evolutionary fitness should be better if
it needs less energy to operate its nervous system. Based on
your answer to part a, what would you expect evolution to
do to the dimensions \(t\) and \(r?\) What other constraints
would keep these evolutionary trends from going too far?
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{cubecaps}{1}{}{27}The figure shows cross-sectional views of two cubical
capacitors, and a cross-sectional view of the same two
capacitors put together so that their interiors coincide. A
capacitor with the plates close together has a nearly
uniform electric field between the plates, and almost zero
field outside; these capacitors don't have their plates very
close together compared to the dimensions of the plates, but
for the purposes of this problem, assume that they still
have approximately the kind of idealized field pattern shown
in the figure. Each capacitor has an interior volume of 1.00
\(\text{m}^3\), and is charged up to the point where its internal
field is 1.00 V/m.

(a) Calculate the energy stored in the
electric field of each capacitor when they are separate. (answer check available at lightandmatter.com)

(b) Calculate the magnitude of the interior field when the two
capacitors are put together in the manner shown. Ignore
effects arising from the redistribution of each capacitor's
charge under the influence of the other capacitor.(answer check available at lightandmatter.com)

(c) Calculate the energy of the put-together configuration. Does
assembling them like this release energy, consume energy, or neither?(answer check available at lightandmatter.com)
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{earthcap}{0}{}{28}Find the capacitance of the surface of the earth, assuming there is an outer spherical “plate” at infinity. (In reality, this outer plate would just represent some distant part of the universe to which we carried away some of the earth's charge in order to charge up the earth.)(answer check available at lightandmatter.com) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{infinite-strip}{1}{}{29}(a) Show that the field found in example 10 on page 576
reduces to \(E=2k\lambda/R\) in the limit of \(L\rightarrow\infty\).

(b) An infinite strip of width \(b\) has a surface charge density \(\sigma\).
Find the field at a point at a distance \(z\) from the strip,
lying in the plane perpendicularly bisecting the strip.
(answer check available at lightandmatter.com)

(c) Show that this expression has the
correct behavior in the limit where \(z\) approaches zero,
and also in the limit of \(z\gg b\). For the latter, you'll need
the result of problem 22a, which is given
on page 932.
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{charged-solid-cyl}{1}{}{30}A solid cylinder of radius \(b\) and length \(\ell\) is uniformly charged with a total charge \(Q\). Find the electric field at a point at the center of one of the flat ends. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{vedgedisk}{2}{}{31}Find the voltage at the edge of a uniformly charged disk. (Define \(V=0\) to be infinitely far from the disk.) (answer check available at lightandmatter.com)\hwhint{hwhint:vedgedisk} \end{homeworkforcelabel}

\begin{homeworkforcelabel}{capenergy}{0}{}{32}Find the energy stored in a capacitor in terms of its capacitance and the voltage difference across it.(answer check available at lightandmatter.com) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{seriescapacitors}{1}{}{33}(a) Find the capacitance of two identical capacitors in
series.

(b) Based on this, how would you expect the
capacitance of a parallel-plate capacitor to depend on the
distance between the plates?
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{complex-trig}{1}{}{34}(a) Use complex number techniques to
rewrite the function \(f(t)=4\sin\omega t+3\cos\omega t\)
in the form \(A\sin(\omega t+\delta)\).(answer check available at lightandmatter.com)

(b) Verify the result using the trigonometric
identity \(\sin(\alpha+\beta)=\sin\alpha\cos\beta+\sin\beta\cos\alpha\).
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{lrcunits}{0}{}{35}
(a) Show that the equation \(V_L=LdI/dt\) has the right units.

(b) Verify that \(RC\) has units of time.

(c) Verify that \(L/R\) has units of time.
\end{homeworkforcelabel}
\begin{homeworkforcelabel}{parallelinductors}{1}{}{36}Find the inductance of two identical inductors in parallel.
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{i-to-the-i}{1}{}{37}Calculate the quantity \(i^i\) (i.e., find its real and imaginary parts).(answer check available at lightandmatter.com) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{strayimpedance}{0}{}{38}The wires themselves in a circuit can have resistance,
inductance, and capacitance. Would “stray” inductance and
capacitance be most important for low-frequency or for
high-frequency circuits? For simplicity, assume that the
wires act like they're in *series* with an inductor or capacitor.
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{lomega}{0}{}{39} Starting from the relation \(V=LdI/dt\) for the voltage difference across an inductor, show that an inductor has an impedance equal to \(L\omega\). \end{homeworkforcelabel}

\begin{homeworkforcelabel}{charged-long-box}{1}{}{40}A rectangular box is uniformly charged with a charge density \(\rho\). The box is extremely long and skinny, and its cross-section is a square with sides of length \(b\). The length is so great in comparison to \(b\) that we can consider it as being infinite. Find the electric field at a point lying on the box's surface, at the midpoint between the two edges. Your answer will involve an integral that is most easily done using computer software. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{charge-gun}{1}{}{41}A hollow cylindrical pipe has length \(\ell\) and radius \(b\). Its ends are open, but on the curved surface it has a charge density \(\sigma\). A charge \(q\) with mass \(m\) is released at the center of the pipe, in unstable equilibrium. Because the equilibrium is unstable, the particle acclerates off in one direction or the other, along the axis of the pipe, and comes shooting out like a bullet from the barrel of a gun. Find the velocity of the particle when it's infinitely far from the “gun.” Your answer will involve an integral that is difficult to do by hand; you may want to look it up in a table of integrals, do it online at integrals.com, or download and install the free Maxima symbolic math software from maxima.sourceforge.net. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{fmradiolrc}{0}{}{42}If an FM radio tuner consisting of an LRC circuit contains a 1.0 \(\mu\text{H}\) inductor, what range of capacitances should the variable capacitor be able to provide?(answer check available at lightandmatter.com) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{rc-par-impedance}{1}{}{43}(a) Find the parallel impedance of a \(37\ \text{k}\Omega\) resistor and
a 1.0 nF capacitor at \(f=1.0\times10^4\) Hz.(answer check available at lightandmatter.com)

(b) A voltage with an amplitude of 1.0 mV drives this impedance at this
frequency. What is the amplitude of the current drawn from the
voltage source, what is the current's phase angle with respect to the
voltage, and does it lead the voltage, or lag behind it?(answer check available at lightandmatter.com)
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{lrc-z-plot}{1}{}{44}A series LRC circuit consists of a 1.000 \(\Omega\) resistor, a
1.000 F capacitor, and a 1.000 H inductor. (These are
not particularly easy values to find on the shelf at Radio Shack!)

(a) Plot its impedance as a point in the complex plane for each of
the following frequencies: \(\omega\)=0.250, 0.500, 1.000, 2.000, and 4.000 Hz.

(b) What is the resonant angular frequency, \(\omega_{res}\),
and how does this relate to your plot?(answer check available at lightandmatter.com)

(c) What is the resonant frequency \(f_{res}\) corresponding to your answer in part b?(answer check available at lightandmatter.com)
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{series-to-parallel}{1}{}{45}At a frequency \(\omega\), a certain series LR circuit has an impedance of \(1\ \Omega+(2\ \Omega)i\). Suppose that instead we want to achieve the same impedance using two circuit elements in parallel. What must the elements be? \end{homeworkforcelabel}

\begin{homeworkforcelabel}{coaxcap}{1}{}{46}(a) Use Gauss' law to find the fields inside and outside an
infinite cylindrical surface with radius \(b\) and uniform
surface charge density \(\sigma\).(answer check available at lightandmatter.com)

(b) Show that there is a discontinuity in the electric field equal to \(4\pi k \sigma\)
between one side of the surface and the other, as there should be (see page 630).

(c) Reexpress your result in terms of the charge per unit
length, and compare with the field of a line of charge.

(d) A coaxial cable has two conductors:
a central conductor of radius \(a\), and an outer conductor of
radius \(b\). These two conductors are separated by an insulator.
Although such a cable is normally used for time-varying signals,
assume throughout this problem that there is simply a DC voltage
between the two conductors.
The outer conductor is thin, as in part c. The inner
conductor is solid, but, as is always the case with a conductor in electrostatics,
the charge is concentrated on the surface. Thus, you can
find all the fields in part b by superposing the fields due
to each conductor, as found in part c. (Note that on a given length of the cable,
the total charge of the inner and outer conductors is zero, so \(\lambda_1=-\lambda_2\),
but \(\sigma_1\ne\sigma_2\), since the areas are unequal.)
Find the capacitance per unit length of such a cable.(answer check available at lightandmatter.com)
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{gauss-const-e}{1}{}{47}In a certain region of space, the electric field is constant (i.e.,
the vector always has the same magnitude and direction).
For simplicity, assume that the field points in the positive \(x\)
direction. (a) Use Gauss's law to prove that there is no charge
in this region of space. This is most easily done by considering
a Gaussian surface consisting of a rectangular box, whose edges
are parallel to the \(x\), \(y\), and \(z\) axes.

(b) If there are
no charges in this region of space, what could be making this
electric field?
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{lc-e-sharing}{1}{}{48}(a) In a series LC circuit driven by a DC voltage (\(\omega=0\)), compare the energy stored in
the inductor to the energy stored in the capacitor.

(b) Carry out the same comparison for an LC circuit that is oscillating freely (without any driving voltage).

(c) Now consider the general case of a series LC circuit driven by an oscillating voltage at an arbitrary
frequency. Let \(\overline{U_L}\) and be the average energy stored in the inductor, and similarly for \(\overline{U_C}\). Define
a quantity \(u=\overline{U_C}/(\overline{U_L}+\overline{U_C})\), which can be interpreted as the capacitor's average share of the
energy, while \(1-u\) is the inductor's average share. Find \(u\) in terms of \(L\), \(C\), and \(\omega\), and sketch
a graph of \(u\) and \(1-u\) versus \(\omega\). What happens at resonance? Make sure your result is consistent with your answer
to part a.(answer check available at lightandmatter.com)

\end{homeworkforcelabel}

\begin{homeworkforcelabel}{solidchargedcylinder}{1}{}{49}Use Gauss' law to find the field inside an infinite cylinder with radius \(b\) and uniform charge density \(\rho\). (The external field has the same form as the one in problem 46.)(answer check available at lightandmatter.com) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{gauss-simple-e}{1}{}{50}(a) In a certain region of space, the electric field is given by
\(\mathbf{E}=bx\hat{\mathbf{x}}\), where \(b\) is a constant.
Find the amount of charge contained within a cubical volume extending
from \(x=0\) to \(x=a\), from \(y=0\) to \(y=a\), and from \(z=0\) to \(z=a\).

(b) Repeat for \(\mathbf{E}=bx\hat{\mathbf{z}}\).

(c) Repeat for \(\mathbf{E}=13bz\hat{\mathbf{z}}-7cz\hat{\mathbf{y}}\).

(d) Repeat for \(\mathbf{E}=bxz\hat{\mathbf{z}}\).
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{gauss-em-wave}{1}{}{51}Light is a wave made of electric and magnetic fields, and the fields are perpendicular to the direction of the wave's motion, i.e., they're transverse. An example would be the electric field given by \(\mathbf{E}=b \hat{\mathbf{x}} \sin cz\), where \(b\) and \(c\) are constants. (There would also be an associated magnetic field.) We observe that light can travel through a vacuum, so we expect that this wave pattern is consistent with the nonexistence of any charge in the space it's currently occupying. Use Gauss's law to prove that this is true. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{charged-cylinder-div}{1}{}{52}This is an alternative approach to problem 49,
using a different technique.
Suppose that a long cylinder contains a uniform charge
density \(\rho\) throughout its interior volume.

(a) Use the methods of section 10.7
to find the electric field inside the cylinder. (answer check available at lightandmatter.com)

(b) Extend your solution to the outside region, using the same
technique. Once you find the general form of the solution,
adjust it so that the inside and outside fields match up at
the surface.(answer check available at lightandmatter.com)
\end{homeworkforcelabel}

\begin{homeworkforcelabel}{divtrans}{1}{}{53}The purpose of this homework problem is to prove that the divergence is invariant with respect to translations. That is, it doesn't matter where you choose to put the origin of your coordinate system. Suppose we have a field of the form \(\mathbf{E}=ax\hat{\mathbf{x}}+by\hat{\mathbf{y}}+cz\hat{\mathbf{z}}\). This is the most general field we need to consider in any small region as far as the divergence is concerned. (The dependence on \(x\), \(y\), and \(z\) is linear, but any smooth function looks linear close up. We also don't need to put in terms like \(x\hat{\mathbf{y}}\), because they don't contribute to the divergence.) Define a new set of coordinates \((u,v,w)\) related to \((x,y,z)\) by

\[\begin{align*}
x &= u + p \\
y &= v + q \\
z &= w + r ,
\end{align*}\]

where \(p\), \(q\), and \(r\) are constants. Show that the field's divergence is the same in these new coordinates. Note that \(\hat{\mathbf{x}}\) and \(\hat{\mathbf{u}}\) are identical, and similarly for the other coordinates. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{div-rot-invariant}{2}{}{54}Using a techniques similar to that of problem 53, show that the divergence is rotationally invariant, in the special case of rotations about the \(z\) axis. In such a rotation, we rotate to a new \((u,v,z)\) coordinate system, whose axes are rotated by an angle \(\theta \) with respect to those of the \((x,y,z)\) system. The coordinates are related by

\[\begin{align*}
x &= u \cos \theta + v \sin \theta \\
y &= -u \sin \theta + v \cos \theta
\end{align*}\]

Find how the \(u\) and \(v\) components the field \(\mathbf{E}\) depend on \(u\) and \(v\), and show that its divergence is the same in this new coordinate system. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{cylindrical-charge-given-field}{1}{}{55}An electric field is given in cylindrical coordinates \((R,\phi,z)\) by \(E_R=ce^{-u|z|}R^{-1}\cos^2\phi\), where the notation \(E_R\) indicates the component of the field pointing directly away from the axis, and the components in the other directions are zero. (This isn't a completely impossible expression for the field near a radio transmitting antenna.) (a) Find the total charge enclosed within the infinitely long cylinder extending from the axis out to \(R=b\). (b) Interpret the \(R\)-dependence of your answer to part a. \end{homeworkforcelabel}

\begin{homeworkforcelabel}{addition-theorem-for-sine}{1}{}{56} Use Euler's theorem to derive the addition theorems that express \(\sin(a+b)\) and \(\cos(a+b)\) in terms of the sines and cosines of \(a\) and \(b\). (solution in the pdf version of the book) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{cube-roots-of-unity}{1}{}{57} Find every complex number \(z\) such that \(z^3=1\). (solution in the pdf version of the book) \end{homeworkforcelabel}

\begin{homeworkforcelabel}{factor-cubic}{1}{}{58} Factor the expression \(x^3-y^3\) into factors of the lowest possible order, using complex coefficients. (Hint: use the result of problem 57.) Then do the same using real coefficients. (solution in the pdf version of the book) \end{homeworkforcelabel}

Apparatus:

3 solenoids

DC power supply

compass

ruler

cut-off plastic cup

At this point you've studied the gravitational field, \(\mathbf{g}\), and the electric field, \(\mathbf{E}\), but not the magnetic field, \(\mathbf{B}\). However, they all have some of the same mathematical behavior: they act like vectors. Furthermore, magnetic fields are the easiest to manipulate in the lab. Manipulating gravitational fields directly would require futuristic technology capable of moving planet-sized masses around! Playing with electric fields is not as ridiculously difficult, but static electric charges tend to leak off through your body to ground, and static electricity effects are hard to measure numerically. Magnetic fields, on the other hand, are easy to make and control. Any moving charge, i.e., any current, makes a magnetic field.

A practical device for making a strong magnetic field is simply a coil of wire, formally known as a solenoid. The field pattern surrounding the solenoid gets stronger or weaker in proportion to the amount of current passing through the wire.

1. With a single solenoid connected to the power supply and laid with its axis horizontal, use a magnetic compass to explore the field pattern inside and outside it. The compass shows you the field vector's direction, but not its magnitude, at any point you choose. Note that the field the compass experiences is a combination (vector sum) of the solenoid's field and the earth's field.

2. What happens when you bring the compass extremely far away from the solenoid?

What does this tell you about the way the solenoid's field varies with distance?

Thus although the compass doesn't tell you the field vector's magnitude numerically, you can get at least some general feel for how it depends on distance.

3. The figure below is a cross-section of the solenoid in the plane containing its axis. Make a sea-of-arrows sketch of the magnetic field in this plane. The length of each arrow should at least approximately reflect the strength of the magnetic field at that point.

Does the field seem to have sources or sinks?

4. What do you think would happen to your sketch if you reversed the wires?

Try it.

5. Now hook up the two solenoids in parallel. You are going to measure what happens when their two fields combine in the at a certain point in space. As you've seen already, the solenoids' nearby fields are much stronger than the earth's field; so although we now theoretically have three fields involved (the earth's plus the two solenoids'), it will be safe to ignore the earth's field. The basic idea here is to place the solenoids with their axes at some angle to each other, and put the compass at the intersection of their axes, so that it is the same distance from each solenoid. Since the geometry doesn't favor either solenoid, the only factor that would make one solenoid influence the compass more than the other is current. You can use the cut-off plastic cup as a little platform to bring the compass up to the same level as the solenoids' axes.

a)What do you think will happen with the solenoids' axes at 90 degrees to each other, and equal currents? Try it. Now represent the vector addition of the two magnetic fields with a diagram. Check your diagram with your instructor to make sure you're on the right track.

b) Now try to make a similar diagram of what would happen if you switched the wires on one of the solenoids.

After predicting what the compass will do, try it and see if you were right.

c)Now suppose you were to go back to the arrangement you had in part a, but you changed one of the currents to half its former value. Make a vector addition diagram, and use trig to predict the angle.

Try it. To cut the current to one of the solenoids in half, an easy and accurate method is simply to put the third solenoid in series with it, and put that third solenoid so far away that its magnetic field doesn't have any significant effect on the compass.

(c) 1998-2013 Benjamin Crowell, licensed under the Creative Commons Attribution-ShareAlike license. Photo credits are given at the end of the Adobe Acrobat version.

[2] Current is a scalar, since the definition
\(I=dq/dt\) is the derivative of a scalar. However, there is a closely related
quantity called the current *density*, **J**, which is a vector, and **J** is
in fact the more fundamentally important quantity.

[3] As in chapter 2,
we use the word “frequency” to mean either \(f\) or \(\omega=2\pi f\)
when the context makes it clear which is being referred to.

[4] I cheated a little. If \(z\)'s argument
is 30 degrees, then we could say \(\bar{z}\)'s was -30, but we could also call it
330. That's OK, because 330+30 gives 360, and an argument of
360 is the same as an argument of zero.

[5] In general, the use of complex number techniques to
do an integral could result in a complex number, but that complex number would
be a constant, which could be subsumed within the usual constant of integration.

[6] A resistor always turns electrical energy into heat. It never
turns heat into electrical energy!

[7] To many people, the word “radiation” implies nuclear
contamination. Actually, the word simply means something that “radiates” outward.
Natural sunlight is “radiation.” So is the light from a lightbulb, or the infrared light
being emitted by your skin right now.

[8] Note that this time “frequency”
means \(f\), not \(\omega\)! Physicists and engineers generally use \(\omega\) because it
simplifies the equations, but electricians and technicians always use \(f\). The 60 Hz
frequency is for the U.S.