# Schrödinger’s Equation in 1-D: Some Examples

*Michael Fowler, UVa. *

### Curvature of Wave Functions

Schrödinger’s equation in the form

$\frac{{d}^{2}\psi (x)}{d{x}^{2}}=\frac{2m(V(x)-E)}{{\hslash}^{2}}\psi (x)$

can be interpreted by saying that the left-hand side, the
rate of change of slope, is the *curvature*
$\u2013$ so the curvature of the function is
proportional to $\left(V\left(x\right)-E\right)\psi \left(x\right).$ This means that if $E>V\left(x\right),$ for $\psi \left(x\right)$ positive $\psi \left(x\right)$ is curving negatively, for $\psi \left(x\right)$ negative $\psi \left(x\right)$ is curving positively. *In both
cases, $\psi \left(x\right)$ is always curving towards the $x$ -axis* -- so, for $E>V\left(x\right),$ $\psi \left(x\right)$ has a kind of stability: its curvature is
always bringing it back towards the axis, and so generating oscillations. The simplest example is that of a constant
potential $V\left(x\right)={V}_{0}<E,$ for which the wave function is $\psi \left(x\right)=A\mathrm{sin}\left(kx+\delta \right)$ with $\delta $ a constant and
$k=\sqrt{\left(2m/{\hslash}^{2}\right)\left(E-{V}_{0}\right)}.$

On the other hand, for $V\left(x\right)>E,$ the curvature is always *away* from the axis. This
means that $\psi \left(x\right)$ tends to diverge to infinity. Only with *exactly* the right initial conditions
will the curvature be just right to bring the wave function to zero as $x$ goes to infinity. (This is possible because as
$\psi \left(x\right)$ tends to zero, the curvature tends to zero,
too.)

For a constant potential ${V}_{0}>E,$ the wave function is $\psi \left(x\right)=A{e}^{\alpha x}+B{e}^{-\alpha x}$,
with $\alpha =\sqrt{\left(2m/{\hslash}^{2}\right)\left({V}_{0}-E\right)}.$ Of course, this wave function will diverge in
at least one direction! However, as we
shall see below, there are situations with spatially varying potentials where
this wave function is only relevant for positive $x,$ and the coefficients *A*, *B* are functions of the
energy -- for certain energies it turns out that $A=0,$ and the wave function converges.

### One Dimensional Infinite Depth Square Well

In an earlier lecture, we considered in some detail the allowed wave functions and energies for a particle trapped in an infinitely deep square well, that is, between infinitely high walls a distance $L$ apart. For that case, the potential between the walls is identically zero so the wave function has the form $\psi \left(x\right)=A\mathrm{sin}\left(kx+\delta \right).$ The wave function $\psi \left(x\right)$ necessarily goes to zero right at the walls, since it cannot have a discontinuity, and must be zero just inside the wall. Even a quantum particle cannot penetrate an infinite wall!

An immediate consequence is that the lowest state cannot
have zero energy, since $k=0$ gives a
constant $\psi \left(x\right)$. Rather, the lowest energy state must have the
minimal amount of bending of the wave function necessary for it to be zero at *both* walls but nonzero in between -- this
corresponds to half a period of a sine or cosine (depending on the choice of
origin), these functions being the solutions of Schrödinger’s equation in the
zero potential region between the walls.
The allowed wave functions (eigenstates) found as the energy increases
have successively 0, 1, 2, … zeros
(nodes) in the well.

### Parity of a Wave Function

Notice that the allowed wave eigenfunctions of the Hamiltonian for the infinite well are symmetrical or antisymmetrical about the center, $\psi \left(x\right)=\pm \psi \left(-x\right).$

We call the operator that reflects a function in the origin
the *parity* operator $P,$ so these eigenstates of the Hamiltonian are *also* eigenstates of the parity operator,
with eigenvalues $\pm 1.$ This is
because the Hamiltonian is itself symmetric: ${d}^{2}/d{x}^{2}$ is even in $x,$ and so is $V\left(x\right),$ so $\left[H,P\right]=0,$ and the two operators can be simultaneously
diagonalized, that is, a common set of eigenstates can be constructed.

### Finite Depth Square
Well

If the potential at the walls is not infinite, the parity operator $P$ will continue to commute with the Hamiltonian $H$ as long as the potential is symmetric, $V\left(x\right)=V\left(-x\right)$.

We take

$$\begin{array}{l}V\left(x\right)={V}_{0},\text{\hspace{1em}}x<-L/2,\\ V\left(x\right)=0,\text{\hspace{1em}}-L/2\le x\le L/2,\\ V\left(x\right)={V}_{0},\text{\hspace{1em}}L/2<x.\end{array}$$

We only need look for solutions symmetric or antisymmetric about the origin. This is important from a practical point of view, because it allows us to integrate Schrödinger’s equation numerically out from the origin in the positive direction: $\psi \left(x\right)$ in the negative direction is fixed by symmetry (or antisymmetry). Since it’s a second-order equation, we need two boundary conditions to get going, for symmetric states, we can take at $x=0,$ for antisymmetric states, $\psi \left(x\right)=0,\text{\hspace{0.17em}}\text{\hspace{0.17em}}{\psi}^{\prime}\left(x\right)=1\text{at}x=0.$ (Of course, we will have to normalize $\psi \left(x\right)$ correctly eventually.)

The numerical strategy is to pick a value for the energy $E,$ choose one of the boundary conditions above and integrate $\psi \left(x\right)$ numerically to a large positive value of $x.$ For almost all values of $E,$ the wave function will be exponentially increasing with $x.$ For the particular values corresponding to bound states, it will be exponentially decreasing.

It is well worth while building up an intuition for this by playing with the spreadsheet accompanying this lecture: the spreadsheet does the numerical integration for any $E$ and well depth, and has a macro to locate the nearest bound state.

### Joining the Wave Functions Inside and Outside of the Well

The numerical method mentioned above works for any symmetric potential. Fortunately, for the square well, an analytic/graphical method is very effective, and provides more insight.

Let us begin by considering how the lowest energy state wave
function is affected by having finite instead of infinite walls. Inside the well, where $V=0,$ the solution to Schrödinger’s equation is
still of cosine form (for a symmetric state). However, Schrödinger’s equation now
has a nonzero solution *inside* the
wall $\left(x>L/2\right)$,
where $V={V}_{0}$:

$-\frac{{\hslash}^{2}}{2m}\frac{d{\text{\hspace{0.05em}}}^{2}\psi (x)}{d\text{\hspace{0.05em}}{x}^{2}}+{V}_{0}\psi (x)=E\psi (x)$,

has two exponential solutions one increasing with $x,$ the other decreasing,

${e}^{\alpha x}\text{and}{e}^{-\alpha x},\text{where}\alpha =\sqrt{2m({V}_{0}-E)/{\hslash}^{2}}$.

We are assuming here that $E<{V}_{0},$ so the particle is bound to the well. We shall find the lowest energy state is always bound in a finite square well, however weak the potential.

Now, Schrödinger’s equation must be valid everywhere,
including the point $x=L/2$.
Since the potential is finite, *the wave
function $\psi \left(x\right)$ and its first derivative must be continuous at
$x=L/2.$ *

Suppose, then, we choose a particular energy $E.$ Then the wavefunction inside the well (taking
the symmetric case) is proportional to $\mathrm{cos}kx,$ where $k=\sqrt{2mE/{\hslash}^{2}}$.
The wave function (*and* its derivative!) must match a sum of exponential
terms at $x=L/2,$ so

$\begin{array}{l}\text{}\mathrm{cos}(kL/2)=A{e}^{\alpha L/2}+B{e}^{-\alpha L/2}\\ -k\mathrm{sin}(kL/2)=\alpha A{e}^{\alpha L/2}-\alpha B{e}^{-\alpha L/2}\end{array}$

Solving these equations for the coefficients $A,B$ in the usual way, we find that in general the
cosine solution inside the well goes smoothly into a linear combination of
exponentially increasing and decreasing terms in the wall. *However,
this cannot in general represent a bound state in the well*. The increasing
solution increases *without limit* as *x* goes to infinity, so since the square
of the wave function is proportional to the probability of finding the particle
at any point, the particle is infinitely more likely to be found at infinity
than anywhere else. It got away! This
clearly makes no sense -- we’re trying to find wave functions for particles
that stay in, or at least close to, the well.
We are forced to conclude that the *only*
exponential wave function that makes sense is the one for which $A$ *is
exactly zero*, so that there is only a *decreasing*
wave in the wall.

### Finding the Bound
State Energies
Graphically

If we demand that the wavefunction decrease exponentially as
*x* goes to infinity, or, in other
words, *require $A$ to be zero*, $k$ must satisfy the condition given be dividing
one of the boundary equations above by the other:

$\mathrm{tan}(kL/2)=\alpha /k$.

This equation cannot be solved analytically, but is easy to solve graphically by plotting the two sides as functions of $k$ (recall $\alpha =\sqrt{2m({V}_{0}-E)/{\hslash}^{2}}$, and $k=\sqrt{2mE/{\hslash}^{2}}$ ) and finding where the curves intersect.

From

${\alpha}^{2}=\frac{2m{V}_{0}}{{\hslash}^{2}}-{k}^{2}\text{wefind}\frac{\alpha}{k}=\sqrt{\frac{2m{V}_{0}}{{\hslash}^{2}{k}^{2}}-1},$

note that this is real only for

$k<\frac{\sqrt{2m{V}_{0}}}{\hslash}.$

(Because if this inequality is *not* satisfied, the particle has enough kinetic energy to get out of
the well!)

Now the condition for a bound state can be written

$\mathrm{tan}(kL/2)=\frac{\alpha}{k}=\sqrt{\frac{2m{V}_{0}}{{\hslash}^{2}{k}^{2}}-1}.$

Cleaning up the appearance of the equation by choosing variables $x=\frac{kL}{2},\text{\hspace{1em}}{a}^{2}=\frac{m{V}_{0}{L}^{2}}{2{\hslash}^{2}},$ and plotting $\mathrm{tan}x\text{and}\sqrt{{\left(\frac{a}{x}\right)}^{2}-1}$ from $x=0$ to $x=a,$ allowed bound state $k$ -values correspond to the points of intersection of the two curves. The bound state energies are then given by $E={\hslash}^{2}{k}^{2}/2m.$

The variable $a$ is a measure of the attractive strength of the well. Here are the two curves for a shallow well ( $a=1$ ):

It is interesting to note that however small $a$ is, the curve $y=\sqrt{{\left(\frac{a}{x}\right)}^{2}-1}$ goes to infinity as $x$ goes to zero, so will always intersect $y=\mathrm{tan}x$: there will always be a bound state.

A deeper well, $a=20,$ gives several bound states:

For the lower energies at least, the allowed $k$$\u2013$values are
approximately linearly spaced, at about $\pi /2,\text{\hspace{0.17em}}3\pi /2,\text{\hspace{0.17em}}5\pi /2,\dots $ so the bound state energies are not far off
the 1, 9, 25,… pattern of the infinitely
deep square well -- remembering that we are only looking at the *even* parity (cosine) solutions!

*Exercise: *Use the spreadsheet with *D*
= 50, *W* = 4 and find all the even
bound state energies. How well do they
fit this pattern? Can you account for
the deviation? Examine the wave functions for the different eigenenergies: note
how far it penetrates the wall, and how much that changes the boundary
condition at the wall from that for an infinite wall. Which one of the bound
state energies is most affected by this, and how is it affected? Would you
expect that from the graphical solution?

The odd parity solutions, sine waves inside the well, can be found by an exactly similar analysis. One difference is that an arbitrarily weak well will not bind an odd parity state. The point is that for a weak potential to bind an even state, it only has to curve the wave function slightly to get from one exponentially decaying to the left to one exponentially decaying to the right. These curves decay very slowly for a weak potential, and give a bound state in which the particle is most likely to be found outside the well. On the other hand, in an odd solution the wave function within the well has to have enough total curvature to fit together two decaying wave functions which have opposite sign. This takes much more bending, and cannot be achieved with a very weak potential.

*Exercise*: Check this last statement, by
considering what fraction of a wavelength of the oscillating wave function
inside the well is necessary to make a connection between the decaying wave
functions in the walls to the left and right.

### The Delta Function Potential

One limiting case of a square well is a very narrow deep well, which can be approximated by a delta function when the range of variation of the wave function is much greater than the range of the potential, so Schrödinger’s equation becomes

$-\frac{{\hslash}^{2}}{2m}\frac{d{\text{\hspace{0.05em}}}^{2}\psi (x)}{d\text{\hspace{0.05em}}{x}^{2}}+\lambda \delta \left(x\right)\psi (x)=E\psi (x)$

with $\lambda $

negative for an attractive potential.

The infinity of the $\delta $ -function cannot be balanced by the finite right hand side, so the wave function must have a discontinuity in slope at the origin.

To find the ground state energy, note first that as a one-dimensional attractive potential there will be a bound state: any change in slope is sufficient to connect an exponentially increasing function coming in from $-\infty $ to a decreasing one going to $+\infty ,$ since the rates of increase and decrease can be arbitrarily slow.

Away from the origin, then, we can take the wave function to be

$\psi \left(x\right)=A{e}^{-\alpha \left|x\right|}$,

the energy of the state being $E=-{\hslash}^{2}{\alpha}^{2}/2m$.

The discontinuity in slope at the origin is just

$\frac{d\psi \left(x=+\epsilon \right)}{dx}-\frac{d\psi \left(x=-\epsilon \right)}{dx}=-2A\alpha $.

To match this with the $\delta $ -function singularity, we integrate the Schrödinger equation term by term from $-\epsilon $ to $+\epsilon $ in the limit of $\epsilon $ going to zero:

$\underset{-\epsilon}{\overset{\epsilon}{\int}}-\frac{{\hslash}^{2}}{2m}\frac{d{\text{\hspace{0.05em}}}^{2}\psi (x)}{d\text{\hspace{0.05em}}{x}^{2}}dx}+{\displaystyle \underset{-\epsilon}{\overset{\epsilon}{\int}}\lambda \delta \left(x\right)\psi (x)}dx={\displaystyle \underset{-\epsilon}{\overset{\epsilon}{\int}}E\psi (x)dx}.$ going to zero.

The $\delta $ -function term must integrate to $\lambda \psi \left(0\right)=\lambda A.$

The first term just gives the discontinuity in slope,

$\underset{-\epsilon}{\overset{\epsilon}{\int}}-\frac{{\hslash}^{2}}{2m}\frac{d{\text{\hspace{0.05em}}}^{2}\psi (x)}{d\text{\hspace{0.05em}}{x}^{2}}dx}=-\frac{{\hslash}^{2}}{2m}{\displaystyle \underset{-\epsilon}{\overset{\epsilon}{\int}}\frac{d}{dx}}\left(\frac{d\psi}{dx}\right)dx=-\frac{{\hslash}^{2}}{2m}{\left[\frac{d\psi}{dx}\right]}_{-\epsilon}^{\epsilon}=\frac{{\hslash}^{2}}{2m}2A\alpha .$

(Remembering $\lambda $ is negative for an attractive potential).

The energy of the bound state is

$$E=-\frac{{\hslash}^{2}{\alpha}^{2}}{2m}=-\frac{m{\lambda}^{2}}{2{\hslash}^{2}}.$$

*Exercise*: rederive this result by taking the limit
of a narrow deep well, tending to a $\delta $ -function, with a cosine wave function inside.

### A Potential Step

Our analysis so far has been limited to real-valued
solutions of the time-independent Schrödinger equation. This is fine for analyzing bound states in a
potential, or standing waves in general, but cannot be used, for example, to
represent an electron traveling through space after being emitted by an
electron gun, such as in an old fashioned TV tube. The reason is that a *real*-valued wave function $\psi \left(x\right)$,
in an energetically allowed region, is made up of terms locally like $\mathrm{cos}kx$ and $\mathrm{sin}kx,$ multiplied in the full wave function by the
time dependent phase factor ${e}^{-iEt/\hslash}$,
giving equal amplitudes of right moving waves ${e}^{i(px-Et)/\hslash}$ and left moving waves ${e}^{-i(px+Et)/\hslash}$. So, for an electron definitely moving to the
right, even the time-independent part of the wave function must necessarily be complex.

Consider an electron of energy $E$ moving in one dimension through a region of zero potential from large negative $x$ and encountering an upward step potential of height ${V}_{0}$ ( ${V}_{0}<E$ ) at the origin $x=0.$ Of course, strictly speaking, the electron should be represented by a wave packet, and hence could not have a precisely defined energy $E,$ but we assume here that it is a very long wave packet, very close to a plane wave, so we take it that the wave function is:

$\psi (x,t)=A{e}^{ikx}{e}^{-iEt/\hslash}$ for *x*
< 0

(A more precise analysis, in which an incoming wave packet is used, can be done by solving for the plane-wave components individually. In the limit of a wavepacket long compared to the de Broglie wavelength, the result is the same as that found here.)

Visualizing the classical picture of a particle approaching a hill (smoothing off the corners a bit) that it definitely has enough energy to surmount, we would perhaps expect that the wave function continues beyond $x=0$ in the form

$\psi (x,t)=B{e}^{i{k}_{1}x}{e}^{-iEt/\hslash}$ for *x*
> 0,

where ${k}_{1}$ corresponds to the slower speed the particle will have after climbing the hill.

Schrödinger’s equation requires that the wave function have
no discontinuities and no kinks (discontinuities in slope) so the $x<0$ and $x>0$ wave functions must match smoothly at the
origin. For them to have the same value, we see from above that $A=B.$ For
them to have the same slope we must have* $kA={k}_{1}B.$ *Unfortunately, the only way to satisfy
both these equations with our above wave functions is to take $k={k}_{1}$ -- which means there is no step potential at
all!

*Question*: what is wrong with the above reasoning?

The answer is that we have been led astray by the depiction
of the particles as little balls rolling along in a potential, with enough
energy to get up the hill, etc.
Schrödinger’s equation is a *wave
equation*. Building intuition about
solutions should rely on experience with waves. We should be thinking about a
light wave going from air into glass, for example. If we do, we realize that at *any* interface *some of the light gets reflected*. This means that our expression
for the wave function for $x<0$ is incomplete, we need to add a *reflected* wave, giving

$\psi (x,t)=A{e}^{ikx}{e}^{-iEt/\hslash}+C{e}^{-ikx}{e}^{-iEt/\hslash}\text{for}x0,$

$\psi (x,t)=B{e}^{i{k}_{1}x}{e}^{-iEt/\hslash}\text{for}x0.$

Now matching the wave function and its derivative at the origin,

$\begin{array}{c}A+C=B\\ k\left(A-C\right)={k}_{1}B.\end{array}$

The fraction of the wave that is reflected

*$R=\frac{{C}^{2}}{{A}^{2}}={\left(\frac{k-{k}_{1}}{k+{k}_{1}}\right)}^{2}.$*

Evidently, the fraction of the wave transmitted

$T=1-R=\frac{4k{k}_{1}}{{\left(k+{k}_{1}\right)}^{2}}$.

*Question*: isn’t the amount transmitted just given
by ${B}^{2}/{A}^{2}$?

The answer is no. The
ratio ${B}^{2}/{A}^{2}$ gives the relative probability of finding a
particle in some small region in the transmitted stream relative to that in the
incoming stream, but the particles in the transmitted stream are moving more
slowly, by a factor ${k}_{1}/k.$ That means that just comparing the densities
of particles in the transmitted and incoming streams is not enough. The physically significant quantity is the *probability current* flowing past a given
point, and this is the product of the density *and* the speed. Therefore,
the transmission coefficient is ${B}^{2}{k}_{1}/{A}^{2}k.$

*Exercise*: prove that even a step *down* gives rise to some reflection.

### Tunneling through a Square Barrier

If a plane wave coming in from the left encounters a step at the origin of height ${V}_{0}>E,$ the incoming energy, there will be total reflection, but with an exponentially decaying wave penetrating some distance into the step. This, by the way, is a general wave phenomenon, not confined to quantum mechanics. If a light wave traveling through a piece of glass is totally internally at the surface, there will be an exponentially decaying electromagnetic field in the air outside the surface. If another piece of glass with a parallel (flat) surface is brought close, some light will “tunnel through” the air gap into the second piece of glass. We are considering here the quantum analogue of this classical behavior.

Suppose then we replace the step with a barrier,

*$V=0$ *for
$x<0,$ call this region *I*

*$V={V}_{0}$ * for $0<x<L,$ this
is region *II*

*$V=0$ *for
$L<x,$ region *III*.

In this situation, the wave function will still decay
exponentially into the barrier (assuming the barrier is thick compared to the
exponential decay length), but on reaching the far end at $x=L,$ a plane wave solution is again allowed, so
there is a nonzero probability of finding the particle beyond the barrier,
moving with its original speed. This phenomenon is called *tunneling*, since in the classical (particle) picture the particle
doesn’t have enough energy to get over the top of the barrier.

The way to solve the problem is to solve the Schrödinger
equation in the three regions, then apply the boundary conditions. Since we are
interested in the probability of a particle getting through the barrier, we do
not need to worry about normalizing the wave function, so for simplicity we
take an incoming wave of unit amplitude.
In region *I*, there will also
be a reflected wave, so

$${\psi}_{I}\left(x\right)={e}^{ikx}+B{e}^{-ikx}.$$

In region *II*,
there will in general be both exponentially decreasing and exponentially
growing solutions, so we take

$${\psi}_{II}\left(x\right)=C{e}^{\alpha x}+D{e}^{-\alpha x}.$$

Recall $\alpha =\sqrt{\left(2m/{\hslash}^{2}\right)\left({V}_{0}-E\right)}.$

In region *III*,
there is only the outgoing wave, to make the equations easy we absorb a phase
factor in the coefficient, and write:

$${\psi}_{III}\left(x\right)=S{e}^{ik\left(x-L\right)}.$$

We now require $\psi \left(x\right)$ and ${\psi}^{\prime}\left(x\right)$ be continuous at $x=0,L.$ Elementary computations lead to

$\begin{array}{c}2ik=(ik+\alpha )C+(ik-\alpha )D\\ 2\alpha C{e}^{\alpha L}=(ik+\alpha )S\\ 2\alpha D{e}^{-\alpha L}=-(ik-\alpha )S.\end{array}$

Solving these equations gives

$S(k)=\frac{2k\alpha}{2k\alpha \mathrm{cosh}\alpha L+i({\alpha}^{2}-{k}^{2})\mathrm{sinh}\alpha L.}$

The probability of tunneling is:

$|S(k){|}^{2}=\frac{4{k}^{2}{\alpha}^{2}}{{({k}^{2}+{\alpha}^{2})}^{2}{\mathrm{sinh}}^{2}\alpha L+4{k}^{2}{\alpha}^{2}}.$

An important limit is that of a barrier thick compared with the decay length, $\alpha L\gg 1.$

In this limit, ${\mathrm{sinh}}^{2}\alpha L\approx {\scriptscriptstyle \frac{1}{4}}{e}^{2\alpha L}$, and using $\alpha =\sqrt{\left(2m/{\hslash}^{2}\right)\left({V}_{0}-E\right)},\text{\hspace{1em}}E={\hslash}^{2}{k}^{2}/2m$, we find

${\left|S\left(k\right)\right|}^{2}\cong 16\left(\frac{E}{{V}_{0}}\right)\left(1-\frac{E}{{V}_{0}}\right){e}^{-2\alpha L}.$

In typical tunneling problems, the far and away dominant term is the ${e}^{-2\alpha L}$, which may differ from unity by many orders of magnitude.

### The Spherically Symmetric Three-Dimensional Problem

The methods developed above for the one-dimensional system
are almost immediately applicable to a very important three-dimensional case: a
particle in a spherically symmetric potential.
A more detailed treatment will be given later -- we restrict ourselves
here to *spherically symmetric *solutions
of Schrödinger’s equation $\psi \left(r,\theta ,\varphi \right)=\psi \left(r\right)$,
a subspace of the space of all possible solutions that always includes the
ground state.

The kinetic energy operator on states in this subspace (where $d/d\theta \equiv 0,\text{\hspace{0.17em}}\text{\hspace{0.17em}}d/d\varphi \equiv 0$ ) is

$\frac{{\overrightarrow{p}}^{2}}{2m}=-\frac{{\hslash}^{2}{\overrightarrow{\nabla}}^{2}}{2m}=-\frac{{\hslash}^{2}}{2m}\frac{1}{{r}^{2}}\frac{d}{dr}\left({r}^{2}\frac{d}{dr}\right).$

It is easy to check that if we write the wave function

$\psi \left(r\right)=\frac{u\left(r\right)}{r}$

the function $u\left(r\right)$ obeys the one-dimensional equation

$-\frac{{\hslash}^{2}}{2m}\frac{{d}^{2}u\left(r\right)}{d{r}^{2}}+V\left(r\right)u\left(r\right)=Eu\left(r\right)$

exactly like a particle in one dimension, except that here $r$ is only positive, and $u\left(r\right)$ must go to zero at the origin. (If $u\left(r\right)$ does *not*
go to zero, *ψ*(*r*) will be at best of order $1/r$ near the origin, and, going back momentarily
to three dimensions, ${\overrightarrow{\nabla}}^{2}\psi \sim \delta \left(\overrightarrow{r}\right)$,
so Schrodinger’s equation will not be satisfied with any realizable potential.)

*Exercise*: for a spherical square well, $V=0\text{if}r{r}_{0},\text{\hspace{1em}}V={V}_{0}\text{for}r\ge {r}_{0}$,
find the minimum value of ${V}_{0}$ for which a bound state exists for given ${r}_{0}$ and particle mass $m.$ Sketch the wave function.

### Alpha Decay

A good example of tunneling, and one which historically helped establish the validity of quantum ideas at the nuclear level, is $\alpha $ -decay. Certain large unstable nuclei decay radioactively by emitting an $\alpha $ -particle, a tightly bound state of two protons and two neutrons. It is thought that $\alpha $ -particles may exist, at least as long lived resonances, inside the nucleus. For such a particle, the strong but short ranged nuclear force creates a spherical finite depth well having a steep wall more or less coinciding with the surface of the nucleus. However, we must also include the electrostatic repulsion between the $\alpha $ -particle and the rest of the nucleus, a potential $(1/4\pi {\epsilon}_{0})(Z-2)2{e}^{2}/r$ outside the nucleus. This means that, as seen from inside the nucleus, the wall at the surface may not be a step but a barrier, in the sense we used the word above, a step up followed by a slide down the electrostatic curve:

Therefore, an $\alpha $ -particle bouncing around inside the nucleus may have enough energy to tunnel through to the outside world.

The $\alpha $ -particles are emitted with spherical symmetry, so the wave function can be written $\psi \left(r\right)=u\left(r\right)/r,$ as discussed above, and Schrödinger’s equation is

$-\frac{{\hslash}^{2}}{2m}\frac{{d}^{2}u\left(r\right)}{d{r}^{2}}+V\left(r\right)u\left(r\right)=Eu\left(r\right),\text{\hspace{1em}}r>0.$

It is evident that the more energetic the $\alpha $ -particle is, the thinner the barrier it
faces. Since the wave function decays
exponentially in the barrier, this can make a huge difference in tunneling
rates. It is not difficult to find the
energy with which the $\alpha $ -particle hits the nuclear wall, because this
will be the same energy with which it escapes. Therefore, if we measure the energy of an
emitted $\alpha $,
since we think we know the shape of the barrier pretty well, we should be able,
at least numerically, to predict the tunneling rate. The only other thing we need to know is how
many times per second $\alpha $ ’s bounce off the wall. The size of the nucleus is of order 10^{-14}
meters (10 fermis), if we assume an $\alpha $ moves at, say, 10^{7} meters per
second, it will bang into the wall 10^{21} times per second. This is a bit handwaving, but all $\alpha $ -radioactive nuclei are pretty much the same
size, so perhaps it’s safe to assume this will be about the same for all of
them.

This is a huge number -- the probability of transmission is evidently very tiny! In other words, the decay length of the wave function inside the barrier is extremely short (except for the very last bit as it emerges into the outside world). It’s so short, in fact, that we can get results in good agreement with experiment by dividing the barrier into a sequence of square barriers and using the above $\alpha L\gg 1$ formula for each of them,

$\psi \left(r+\Delta r\right)\approx \psi \left(r\right){e}^{-\alpha \left(r\right)\Delta r}$

(neglecting the slowly varying and completely unimportant $1/r$ term) so the total attenuation of the wave function in this approximation is the product of terms like this,

$\begin{array}{c}\psi \left(\text{exit}\right)=\psi \left(\text{nucl}\right){\displaystyle \prod _{i}{e}^{-\alpha \left({r}_{i}\right)\Delta r}}\\ \approx \psi \left(\text{nucl}\right){e}^{-{\displaystyle \int \alpha \left(r\right)dr}}\\ =\psi \left(\text{nucl}\right){e}^{-{\displaystyle \int \sqrt{\left(2m/{\hslash}^{2}\right)V\left(r\right)-E}\text{\hspace{0.17em}}dr}}\end{array}$

Since we know the actual shape of the barrier, this integral can be done with elementary functions, and the result for the transmission rate is

${\left|S\left(k\right)\right|}^{2}\approx A{e}^{-B/\sqrt{E}}.$

Here $B=\left(\pi \sqrt{2m}/\hslash \right)\left(Z-2\right)2{e}^{2}$ is *not*
an adjustable parameter: and plotting $\mathrm{ln}{\left|S\left(k\right)\right|}^{2}$ against $1/\sqrt{E}$ for Polonium^{212} (which emits $\alpha $ ’s with energy 8.95MeV, and lasts $3\times {10}^{-7}$ seconds) Thorium^{232} (4.05MeV $\alpha $ ’s, $1.4\times {10}^{10}$ years), and several intermediate lifetime
nuclei gives a straight line plot with the correct slope within a few percent! These elements can all be understood in terms
of essentially the same barrier being tunneled through at the different heights
corresponding to the $\alpha $ energy.

The treatment here is a slightly simplified version of the WKB method, to be discussed in detail later. Further refinements make little difference to the final result in this case.

*Source*:
many of the topics covered in this lecture are elementary, and treated in any
quantum textbook. For some of them I’ve
followed (more or less) the excellent book by French and Taylor, *An Introduction to Quantum Physics*, Norton, 1978.