Time-Dependent Solutions: Propagators and Representations
Michael Fowler, UVa
We’ve spent most of the course so far concentrating on the eigenstates of the Hamiltonian, states whose time-dependence is merely a changing phase. We did mention much earlier a superposition of two different energy states in an infinite well, resulting in a wave function sloshing backwards and forwards. It’s now time to cast the analysis of time dependent states into the language of bras, kets and operators. We’ll take a time-independent Hamiltonian with a complete set of orthonormalized eigenstates, and as usual
Or, as we would now write it
Since is itself time independent, this is very easy to integrate!
The exponential operator that generates the time-dependence is called the propagator, because it describes how the wave propagates from its initial configuration, and is usually denoted by
It’s appropriate to call the propagator , because it’s a unitary operator:
Since is Hermitian, is unitary. It immediately follows that
the norm of the ket vector is conserved, or, translating to wave function language, a wave function correctly normalized to give a total probability of one stays that way. (This can also be proved from the Schrödinger equation, of course, but this is quicker.)
This is all very succinct, but unfortunately the exponential of a second-order differential operator doesn’t sound too easy to work with. Recall, though, that any function of a Hermitian operator has the same set of eigenstates as the original operator. This means that the eigenstates of are the same as the eigenstates of , and if then
This is of course nothing but the time dependent phase factor for the eigenstates we found beforeand, as before, to find the time dependence of any general state we must express it as a superposition of these eigenkets, each having its own time dependence. But how do we do that in the operator language? Easy: we simply insert an identity operator, the one constructed from the complete set of eigenkets, thus:
Staring at this, we see that it’s just what we had before: at the initial time the wave function can be written as a sum over the eigenkets:
with , , and the usual generalization for continuum eigenvalues, and the time development is just given by inserting the phases:
The expectation value of the energy in ,
and is (of course) time independent.
The expectation value of the particle position x is
and is not in general time-independent. (It is real, of course, on adding the term to the term.)
This analysis is only valid for a time-independent Hamiltonian. The important extension to a system in a time-dependent external field, such as an atom in a light beam, will be given later in the course.
The Free Particle Propagator
To gain some insight into what the propagator looks like, we’ll first analyze the case of a particle in one dimension with no potential at all. We’ll also take to make the equations less cumbersome.
For a free particle in one dimension the energy eigenstates are also momentum eigenstates, we label them , so
Let’s consider (following Shankar and others) what seems the simplest example.
Suppose that at , a particle is at : : what is the probability amplitude for finding it at at a later time ? (This would be just its wave function at the later time.)
On examining the above expression, though, it turns out to be nonsense! Noting that the term in the exponent is pure imaginary, independent of ! This particle apparently instantaneously fills all of space, but then its probability dies away as
Question: Where did we go wrong?
Answer: Notice first that is constant throughout space. This means that the normalization, ! And, as we’ve seen above, the normalization stays constant in timethe propagator is unitary. Therefore, our initial wave function must have had infinite norm. That’s exactly rightwe took the initial wave function .
Think of the -function as a limit of a function equal to over an interval of length , with going to zero, and it’s clear the normalization goes to infinity as . This is not a meaningful wave function for a particle. Recall that continuum kets like are normalized by , they do not represent wave functions individually normalizable in the usual sense. The only meaningful wave functions are integrals over a range of such kets, such as . In an integral like this, notice that states within some tiny -interval of length say, have total weight , which goes to zero as is made smaller, but by writing we took a single such state and gave it a finite weight. This we can’t do.
Of course, we do want to know how a wave function initially localized near a point develops. To find out, we must apply the propagator to a legitimate wave functionone that is normalizable to begin with. The simplest “localized particle” wave function from a practical point of view is a Gaussian wave packet,
(I’ve used in place of Shankar’s here to try to minimize confusion with etc.)
The wave function at a later time is then given by the operation of the propagator on this initial wave function:
The integral over is just another Gaussian integral, so we use the same result,
Looking at the expression above, we can see that
where the second exponential is the term . As written, the small limit is not very apparent, but some algebraic rearrangement yields:
It is clear that this expression goes to the initial wave packet as goes to zero. Although the phase has contributions from all three terms here, the main phase oscillation is in the third term, and one can see the phase velocity is one-half the group velocity, as discussed earlier.
The resulting probability density:
This is a Gaussian wave packet, having a width which goes as for large times, where is the width of the initial packet in -spaceso is the spread in velocities within the packet, hence the gradual spreading in -space.
It’s amusing to look at the limit of this as the width of the initial Gaussian packet goes to zero, and see how that relates to our -function result. Suppose we are at distance from the origin, and there is initially a Gaussian wave packet centered at the origin, width At time , the wave packet has spread to and has of order at Thereafter, it continues to spread at a linear rate in time, so locally must decrease as to conserve probability. In the -function limit , the wave function instantly spreads through a huge volume, but then goes as as it spreads into an even huger volume. Or something.
Schrödinger and Heisenberg Representations
Assuming a Hamiltonian with no explicit time dependence, the time-dependent Schrödinger equation has the form
and as discussed above, the formal solution can be expressed as:
Now, any measurement on a system amounts to measuring a matrix element of an operator between two states (or, more generally, a function of such matrix elements).
In other words, the physically significant time dependent quantities are of the form
where is an operator, which we are assuming has no explicit time dependence.
So in this Schrödinger picture, the time dependence of the measured value of an operator like or comes about because we measure the matrix element of an unchanging operator between bras and kets that are changing in time.
Heisenberg took a different approach: he assumed that the ket describing a quantum system did not change in time, it remained at but the operators evolved according to:
Clearly, this leads to the same physics as before. The equation of motion of the operator is:
The Hamiltonian itself does not change in timeenergy is conserved, or, to put it another way, commutes with But for a nontrivial Hamiltonian, say for a particle in one dimension in a potential,
the separate components will have time-dependence, parallel to the classical case: the kinetic energy of a swinging pendulum varies with time. (For a particle in a potential in an energy eigenstate the expectation value of the kinetic energy is constant, but this is not the case for any other state, that is, for a superposition of different eigenstates.) Nevertheless, the commutator of will be time-independent:
(The Heisenberg operators are identical to the Schrödinger operators at )
Applying the general commutator result ,
and since ,
This result could also be derived by writing as an expansion in powers of then taking the commutator with
Exercise: check this.
Notice from the above equations that the operators in the Heisenberg Representation obey the classical laws of motion! Ehrenfest’s Theorem, that the expectation values of operators in a quantum state follow the classical laws of motion, follows immediately, by taking the expectation value of both sides of the operator equation of motion in a quantum state.
Simple Harmonic Oscillator in the Heisenberg Representation
For the simple harmonic oscillator, the equations are easily integrated to give:
We have put in the subscript to emphasize that these are operators. It is usually clear from the context that the Heisenberg representation is being used, and this subscript may be safely omitted.
The time-dependence of the annihilation operator is:
Note again that although is itself time-independent, it is necessary to include the time-dependence of individual operators within
Actually, we could have seen this as follows: if are the energy eigenstates of the simple harmonic oscillator,
Now the only nonzero matrix elements of the annihilation operator between energy eigenstates are of the form
Since this time-dependence is true of all energy matrix elements (trivially so for most of them, since they’re identically zero), and the eigenstates of the Hamiltonian span the space, it is true as an operator equation.
Evidently, the expectation value of the operator in any state goes clockwise in a circle centered at the origin in the complex plane. That this is indeed the classical motion of the simple harmonic oscillator is confirmed by recalling the definition , so the complex plane corresponds to the phase space discussed near the beginning of the lecture on the Simple Harmonic Oscillator. We’ll discuss this in much more detail in the next lecture, on Coherent States.
The time-dependence of the creation operator is just the adjoint equation: