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ROBERT FIELD: OK.
So this is going to be a fun lecture because it's mostly
pictures and language.
And it's also an area of physical chemistry,
which is pretty much--
I mean, there's three areas of physical chemistry
where people have trouble talking to each other.
There's statistical mechanics.
There's quantum mechanics.
And there's the time dependent, time independent forms
of quantum mechanics.
And these three communities have to learn
how to talk to each other.
And I'm hoping that I will help to bridge that gap.
OK.
So last time, we talked about the time dependent Schrodinger
equation.
It's a simple looking little thing.
Remember though, it's an extra level of complexity
on what you already understand.
Now, in the special case where the Hamiltonian is time
independent, then, if you know all of the energy levels
and wave functions for the time independent Hamiltonian,
you can immediately write down the solution
to the time dependent Hamiltonian.
And so you have a complete set of wave functions.
And you have a complete set of energy levels.
And with that, you can basically describe something
that satisfies this thing.
Another set of coefficients is often something
that you arrange for simplicity or for insight.
And I want to understand--
I want to talk about that.
OK.
And so in the previous lecture, we
talked about the probability density, which is psi star psi.
And that can move.
And that can move in two ways.
In the wave function, if there are two or more states
belonging to two or more different energies,
then you can have motion.
And you can have motion like breathing, where probability
moves towards the extremes, or motion
where there is actually a wave packet going from one side
to another.
So for anything interesting to happen,
this probability density has to include
at least two different eigenstates belonging
to two different energy levels.
Now, the total probability is just the integral
over all coordinates of the probability density.
And probability is conserved.
So one of the things that happens--
when you do an integral, the wave functions go away.
And in this particular case, integral psi star psi,
all you get is one.
Or you get a constant, depending on how you normalize things.
But it's not time dependent.
Now, in understanding motion from classical mechanics,
we know Newton's equations.
We know how the coordinate and the momentum depend on time.
And so if we calculate the expectation
value of the coordinate or the expectation
value of the momentum, we get some results.
And it turns out that these things describe the motion
of the center of a wave packet.
A wave packet is anything that's not just a single eigenstate,
so it moves.
And so the motion of a single eigenstate--
the motion of a wave packet is described by Newton's laws.
And this is Ehrenfest theorem.
And it can easily be proven.
But we're not going to prove it.
We're just going to use it.
So we are very interested in expectation values
of the coordinate and the momentum.
And for a harmonic oscillator, this is duck soup.
Then we have nothing but trivial integrals involving
the a's and a-daggers.
And so even though in some ways the harmonic oscillator
is a more complicated problem than the particle in a box,
the harmonic oscillator is the problem
of choice for dealing with motion and developing insight.
There's another useful--
OK.
We have this wave function here.
There is a huge amount of information embedded in it,
too much to just look at.
We need to have ways of reducing that information.
And one of the nice ways is the survival probability.
The survival probability tells you
how fast does the initial state move away from itself.
And this is very revealing.
Another very revealing thing is if this survival probability,
which is a function of time and nothing
else, because we've integrated over the wave functions--
if this survival probability goes up and down
and up and down, there are recurrences.
So at a maximum, which is usually
a maximum at t equals 0 because the wave function is it
at its birthplace, the survival probability
will start high and go down, and come up, and go down.
And there's all sorts of information about recurrences.
As the wave function returns to its birthplace,
it might not return completely.
And so we get partial recurrences.
And these tell us something.
And the times at which the maxima in the survival
probability occur tell us a lot about the potential.
And there are some grand recurrences
where, because all of the energy level differences
are an integer multiple of a common factor,
then you get a perfect recurrence.
And these are wonderful for drawing pictures.
Now, you really want to understand the concepts of time
dependent quantum mechanics pictorially
and to develop a language that describes it.
And there are a lot of little pieces
here that you need to convince yourself you understand
so you can use the language.
OK.
One of the things I said at the beginning of the course
is the central object in quantum mechanics is the wave function.
Or we could generalize to this.
This is actually the truth.
This is a partial truth.
This is everything that we can possibly know.
But we can't know this.
We can never observe the wave function.
However, we do observations.
And we construct a picture, which
is what we call the effective Hamiltonian.
This effective Hamiltonian describes everything
we know, mostly energy levels.
We have formulas for the energy levels.
And we determine the constants.
There's all sorts of stuff that we collect by experiment.
And so we create an object which we think
is like the true Hamiltonian.
And by having the effective Hamiltonian,
we can get these things.
So we observe we make some observations.
And then this is a reduced version of the truth.
And we can get a pretty good representation
of the thing that is supposedly hidden from us.
OK.
So let's start now at t equals 0.
At t equals 0, which I like to call the pluck--
and it really makes it contact with those of you who
are musicians, that you know how to create
a particular kind of sound, which will evolve in time.
And it depends on the details of how you handle the instrument.
So at t equals 0, we have this thing
which, if we have a complete set of eigenfunctions
of the Hamiltonian, of the time independent Hamiltonian,
we know we can write this as cj psi j of x.
Now, often we don't need an infinite number of terms.
But we know that there are lots of different kinds of plucks.
And you can find out what these coefficients are
by just calculating overlap integral of these functions
with this initial state.
OK.
So this is telling you what happens at t equals 0.
And if you can write the initial state
as a superposition of eigenstates,
then you can immediately write the time
evolving object this way.
Now, we have a minus i.
Well, why do we need a minus i?
Well, because we're going to take
the time derivative of the Hamiltonian
and multiply it by iH bar.
We're going to want to get the energy, not minus the energy.
And so we need a minus i here.
And we need a divided by H bar here
in order to satisfy the time independence or time
dependence.
So this always bothers people.
Why should there be an i here?
And why should it be minus i?
And I recommend not trying to memorize it,
but to just convince yourself.
I need the minus i because I'm going to bring down a minus i
over H bar times e.
And we have this iH bar.
The minus i times i gives plus 1.
OK.
So now, in understanding how the time dependent Hamiltonian can
be sampled, we build the superposition states
with a minimum number of terms, like two or three.
Even though, in order to create a very, very sharply localized
state, it needs a huge number of terms here.
But you always build your insight
with something you can do in your head.
And so for some problems, you need only two states.
And for others, you need three.
And those are the ones you want to kill.
You want to understand everything
you can build with two and three state superpositions.
OK.
So there's two classes of problems.
OK so for a half harmonic oscillator--
so for a half harmonic oscillator,
we start with harmonic oscillator
and divide it in half and say this goes to infinity.
And so this side is not accessible.
And so if the potential is half of a harmonic oscillator
potential, then we know immediately what
the eigenvalues and eigenfunctions are.
They are the harmonic oscillator functions
that have a node in the middle.
So we know that we have v equals 1, v equals 3.
No v equals 0 or 2.
I mean, this corresponds to the lowest level, v
equals 0 for the half oscillator.
But this is basically-- now, what
we're going to do is we create some state of a half
oscillator.
And then we take away the barrier.
So that's a cheap way of creating localization.
Of course, we can't do this experimentally.
But you could, in principle, do it.
And so basically, you want an initial state,
which is a superposition of vibrational levels.
OK.
And this initial state needs to have the wave
function be 0 at the barrier.
So since we're going to be looking at the full potential,
we're taking away the barrier.
We're allowed to use the even and odd states.
And so let's take the three lowest states.
And so we have c0 psi 0 plus c1 psi 1 plus c2 psi 2.
OK.
This guy is OK.
Yes?
AUDIENCE: When you create the states of the half harmonic
oscillator, do you have to re-scale them
so that they normalize?
ROBERT FIELD: Yes.
We play fast and loose with normalization constants.
We already always know that, whenever
you want to calculate anything, you're
going to divide by the normalization integral.
However, it's OK.
Because we're going to be using the full harmonic oscillator
functions, which do exist over here.
And it's fine once we remove the barrier.
But we want to choose a problem which is as simple as possible.
OK, now, this guy is not 0 at x equals 0.
And this guy is not 0 at x equals 0.
But you can say 0 is equal to c0 psi 0 of 0 plus c2 psi 2 of 0.
We choose the coefficients so that these two guys together
make 0 at the boundary.
And why do we do this?
We're going to be calculating expectation values of x and p.
And if we only have half of the energy levels,
all of the intricacies are going to be 0.
So we have to have three consecutive levels
to have anything interesting.
OK, so the artifice of making these two--
arranging the coefficients so that you get a temporary node
at x equals 0--
it won't stay a node.
Because when we let things oscillate with time,
these two will oscillate differently.
And the node will go away.
But that's how you do it.
That's how you build a superposition.
OK.
Now, what we want to do is to be able to draw pictures
of what's happening and also to calculate what's going on.
And one of the things we use for our pictures
is the expectation value of x and the expectation value of p.
So you know how to calculate the expectation value of x.
We have this capital psi star x capital psi star capital
psi integrate over x.
And so we get to c0 c1 x01 cosine omega t plus 2
c1 c2 x12 cosine omega t.
Now, how did I do that?
Oh, come on.
You can do it, too.
So what is this x01?
Well, x01 is the integral psi 0 star x psi 1 dx.
And we know we can replace x by a plus a-dagger
times the constant.
We always like to forget that concept.
We only bring it in at the end anyway.
And so, well, this has a value--
it's a constant, the constant that we're forgetting--
times 1 square root, right?
And x12 is the same sort of thing.
It's going to be the same constant times 2 square root.
This is easy.
So getting from this symbol to this,
that just requires a little practice,
and then simplifying further to know
what these x's are, and then the constraints on c2 and c0.
We have all that stuff.
OK.
And now, we can draw a picture of what's going to happen.
So here we have the full oscillator.
And let's just draw some energy which is--
now that's complicated.
We have a time dependent wave function,
which is composed of several different energy eigenstates.
So what is its energy?
Well, you can evaluate what the energy
is by taking the expectation value of the Hamiltonian.
And so you can do that.
So what we've made at t equals 0 is
something that looks like this.
It's localized on the left side.
Or it's more localized on the left side.
Now, sometimes, you're going to worry about phase.
And so many times when you're working symbolically
rather than actually evaluating integrals,
there are symbolic phase choices that what you're using
has made.
And for example, for the harmonic oscillator,
if you look in the book, you'll see
that, for all of the harmonic oscillator functions,
the outer lobe is always positive.
And the inner lobe is alternating
with the quantum number.
So that's a phase convention that's implicit in everything
that people have derived.
And as long as the different things
you combine in doing a calculation involve
the same phase convention, which is implicit-- we don't
want to look at what functions.
We want to look at these xij's.
OK.
And so those things that we're manipulating
have a phase implicit in how you define them.
But that's gone in your manipulation.
So you want to be a little careful.
OK.
So we start out and the expectation value
is on this side.
And the psi star psi is localized on this side mostly.
And at a later time--
so this is a later time.
I shouldn't make it bigger.
At a later time, this thing has moved to the other turning
point.
Back and forth, back and forth.
Now, since we have three energy levels--
and well, actually, we have a coherence term
which involves the product of psi 0 and psi 1
and psi 1 and psi 2--
they differ in energy both by omega.
So these two things have the same oscillation frequency.
And so what's going to happen is the wave function, the wave
packet, is going to move from this side to that side,
back and forth always forever at the same frequency,
no dephasing.
In the middle, I can't tell you what it's going to look like.
I don't want to tell you.
Because you don't care.
You care mostly about what's it going to look like at a turning
point.
Or what is it going to look like when it returns to home base?
And all sorts of insights come from that.
OK.
Now, I said, well, if we want to know the energy of this wave
packet, well, we take the expectation value
of the Hamiltonian.
And the expectation of the Hamiltonian
is c0 squared e0 plus c1 squared e1 plus c2 squared e2.
These things are easy once you've gone
through it a couple of times.
Because what's happening is you have these factors,
e to the minus i ej t over H bar.
And they cancel when you do a psi star psi.
Or they generate a difference, omega H bar omega,
when you have different values of the energy.
So this is something that you can derive really quickly.
And the fact that your eigenfunction--
the psi's in your linear combination
up there are eigenfunctions of the Hamiltonian.
So every time the Hamiltonian operates in a wave function,
it gives the energy times that wave function.
And then you're taking the expectation value.
And so we have the wave function time itself integrated.
And that goes away.
So after doing this a few times, you
don't need to write the intermediate steps.
And you shouldn't.
Because you'll get lost in the forest of notation.
Because one of the things you probably
noticed in the last lecture is the equations got really big.
And then we calculate something else.
And it gets twice as big.
And then all of a sudden, it all goes away.
And that's what you want to be able to anticipate.
OK.
So you can really kill this half oscillator problem.
There's nothing much happening except you
create a localization.
And when you take away the other--
when you restore the full oscillator,
everything oscillates at omega.
And so you have a whole bunch of terms
contributing to the motion of the wave packet.
And they're all very simple.
Because they're all oscillating at the same frequency.
Now, as an aside, I want to say there's a huge number of stuff
that's up in this lecture that's going to be
on the exam, a huge amount.
So if for example you wanted to calculate something
like x squared, well, fine.
You know what the selection rule for x squared is.
It's delta v of 0 plus or minus 2.
And so this thing is going to generate some constant terms
and some terms at 2 omega.
OK.
So there are a lot of things about the harmonic oscillator
that make it really wonderful to consider a problem, even
a complicated problem, which is not explicitly
a harmonic oscillator problem.
Because you can get everything so quickly without any
thought after a little bit of investment.
OK.
Now, we haven't talked about electronic transitions
and potential energy curves.
But we will.
And I think you know about them.
And so we have some electronic ground state.
And we have some electronically excited state.
And so each of these states has a vibrational coordinate.
And we can pretend that it's harmonic even if it's not.
Because we build a framework treating
them as harmonic, and then discover
that there's discrepancies which we can fit to a model.
And we can determine from the time
dependence what that model is.
OK.
So we start out with a molecule in v equals 0.
And there is a much repeated truism.
Electrons move fast, nuclei slow.
Transition is instantaneous, or nearly instantaneous,
because it involves the electrons.
So what ends up happening is you draw a vertical line.
And now, you transfer this wave function to the upper state.
You just move-- this is the probability amplitude
distribution of the vibration.
We transfer that to the excited state.
And that's not an eigenstate, the excited state.
It's a localized state, localized at a turning point.
Now, you want to know--
so there's the Franck-Condon principle,
that is just another way of saying electrons
move fast, nuclei slow.
And there is delta x equals 0 delta p equals 0.
If the nuclear state can't change while the electron is
jumping, then the coordinate and the momentum are both constant.
So you're creating a wave packet.
And the best place to create it is near a turning point.
Because then, you can match the momentum of this guy
to that zero point momentum, which you can calculate.
You know how to calculate this.
Because the potential energy curve is 1/2 k x squared.
And the momentum is given by this energy difference here.
And so you can work it out.
It's in the notes.
I don't want to write it down.
So you're going to create something
which is vertical and is not quite exactly
at the turning point.
Because you have to have a little bit of momentum
to match the zero point momentum here.
So you know everything about the initial state.
And so you can calculate what it is by taking the overlap of v
equals 0 of the ground state with all
of the vibrational levels of the excited state.
And so we have the coefficients of each
of those vibrational levels in the excited state that
makes this wave packet.
Now, of course, this wave packet is
going to move back and forth, back and forth.
And if this were a harmonic oscillator,
it would move harmonically.
And so the only thing that would appear
in the expectation value of x is going
to be this motion at omega.
Now, this is usually a relatively high
vibrational level.
And the molecule is not being harmonic here.
So there are correction terms called anharmonicity terms.
So we have the energy level expression plus H bar omega e
xe--
that's one number-- plus 1/2 squared.
So we have a linear term and a quadratic term.
And this omega e xe is on the order of 0.02 times omega
e, 2%.
So it's a small thing.
But if you're going to be allowing a wave
packet to be built out of many vibrational levels,
this guy is going to de-phase a little bit.
So you go around and come back.
And you can't quite have everybody
back where they started.
And so you'll see a decreasing amplitude here.
And that's best looked at by the survival probability.
And you'll see characteristic behavior in the survival
probably.
OK.
But let's go a little bit deeper before I
move on to-- what time is it?
Oh, I'm doing OK.
So let's just say our superposition
state, the electronically excited state,
is a combination of v equals 10 and v equals 11.
So we know immediately that psi star t psi t--
this probability amplitude-- probability, yes,
this probability is c10 squared psi 10
squared plus c11 squared psi 11 squared plus 2 c10 c11
psi 10 psi 11 cosine omega t.
That's not very legible.
Now, I'm playing fast and loose here.
Because I've done this before.
I know what disappears.
And I know, if it's harmonic, you just get this.
Well, if there's two states, this thing
is really just the frequency associated
with these two levels.
OK.
Now, once we have this, we can also generate the survival
probability.
Well, the survival probability, capital P
of t, that's defined as the square modulus of psi star xt
psi x0 dx.
OK.
And you can immediately write what that is going to be.
It's going to be c10 squared.
And we've integrated so the wave functions go away.
And so we have c10 e to the i H bar 10.5 omega
t divided by H bar plus c11 squared e to the minus i plus H
bar 11.5 omega e over H bar.
OK.
Why did I made the mistake here?
Well, we have a psi star.
And so we're going to get the complex conjugate of e
to the minus i omega.
So you end up getting this.
Practice that.
AUDIENCE: That whole thing is [? the ?]
modulus squared, right?
ROBERT FIELD: Yes.
I have that right.
Exactly.
So and now, lo and behold, we know what to do with this too.
And so we're going to get c1 0 to the 4 plus c--
not 1-0, 10, c11 to the 4 plus 2 c10
squared c11 squared cosine omega t.
Isn't that neat?
So we've got a whole bunch of constant terms.
This is constant.
Because it's square modulus and it's to the fourth power.
And so all of these coefficients are positive.
At t equals 0, this is 1.
And so at t equals 0, the survival probability
is at a maximum.
And at some later time, that survival probability
will be at a minimum.
OK.
And so you can say the maximum will occur at integer when
omega t is equal to 2 n pi.
So then the exponential factor is always 1.
And we have a minimum when omega t is an odd multiple of pi.
And all the exponential factors are minus 1.
So we can also now look at the expectation
value for x of t and p of t.
And I'm going to just draw sketches.
So for x of t, we have something that looks like this.
This is at the left turning point.
This is the right turning point, or near the right
turning point.
And this is at pi over 2 omega.
This is at pi over omega.
So that's the half oscillator point.
Now, it starts out and the expectation value
is at the left turning point.
And it's not changing.
The derivative of the expectation value
with respect to t is 0.
The momentum, which has a different phase--
the momentum starts out at 0 also.
And at pi over 2 omega, it reaches a maximum.
And at pi over omega, it reaches 9 again.
But the important thing here is at t
equals 0 the derivative of the momentum
is as big as it can get.
So what's that telling you?
It's telling you this wave packet,
as far as coordinate space is concerned, it's not moving at t
equals 0.
As far as momentum is concerned, it's moving like crazy.
And so this survival probability is changing entirely dominated
by the change in momentum, which is encoded in the wave
function, which is neat.
Because Newton's equation says that the time derivative
of the momentum is equal to--
that's the mass times acceleration--
is equal to the force, which is minus
the gradient of the potential--
the function of time.
And for a harmonic oscillator, the gradient potential is x kx.
And so it's telling you that we have this relationship
between x and t and p.
And we know what the momentum is.
And I'm sorry.
And so the change in the momentum,
which is responsible for the change in the survival
probability at t equals 0, is due to the gradient
of the potential.
So we're actually sampling what is
the gradient of the potential at the left turning point.
And often, for any kind of a problem,
we want to know what kind of force
is acting on the wave packet.
There it is, classic mechanics embedded in quantum mechanics.
It's really amazing.
So if you have some way of measuring
the survival probability near t equals 0,
it's telling you what the slope of the potential
is at the turning point.
OK.
Well, if we have an initial state which
involves many eigenstates, the Hamiltonian,
we still know that there's going to be some complicated behavior
which is modulated by omega.
So we have a cosine omega t always.
And so no matter what kind of a wave
function we make, if we start out at one turning point,
it's going to go to the other turning point.
And it'll keep coming back, and back, and back.
And so one could imagine doing an experiment where--
let's just draw the excited state and some other repulsive
state.
So at this turning point, vertical transition
to that repulsive state is within the range of your laser.
And at this turning point, it's way high.
And so what you can imagine doing
is probing where this wave packet is as a function of time
by having a probe pulse which creates dissociating fragments.
And now, that is what Ahmed Zewail did.
He talked about real dynamics in real time.
So when the wave packet is here, it can't be dissociated.
When it's here, it can.
And you look at the fragments.
Very simple.
So there are lots of ways of taking these simple pictures
of wave packets moving and saying,
OK, I can use them to set up an experiment where
I ask a very specific question.
And I get answers.
And I know what to do with the answers.
Now, if it's not harmonic, you can still
do Zewail's experiment or some other experiment.
And you can ask, OK, the wave packet moved over here.
And there's some dynamics that occurs.
It dissociates or you do something.
And when it comes back, it's not at the same amplitude.
And so you can use the time history of these recurrences
if it's harmonic.
If it's not harmonic, then the recurrences-- even if nothing
happens over here, the recurrences
will be increasingly less perfect.
And so you measure the anharmonicity.
OK.
Five minutes.
Tunneling is a quantum mechanical phenomenon.
And again, you want to use the simplest possible picture
to understand the signature of tunneling.
And so what do you do?
Well, the simplest thing you can do
is start with a harmonic oscillator.
The next thing you do is you put a barrier in the middle.
And you make it really thin.
Thin is because you don't want to calculate the integral.
You want to just say, oh yeah, I know that the wave function--
forget about the barrier.
We know the magnitude of the wave function at the barrier,
OK?
And so if you have a state which has a maximum here,
well, that means that it's feeling the barrier.
And so you know what to do.
If there is a node here, it doesn't know about the barrier.
So you can do all sorts of things really fast.
OK.
So and it's harmonic because you're going to want to use
a's and a-dagger's.
So v equals 1, 3, 5.
They have nodes here.
They don't know about the barrier.
Or if they do, it's a very modest effect.
If you make this thin enough, you won't know about it all.
And then v equals 0, 2, 2 4, et cetera--
well, they're maxima.
Well, they have a local maximum here.
And remember, this is a harmonic oscillator.
So the big lobes are on the extremes.
The smallest lobe is in the middle, but it's not 0.
OK.
There are also symmetry restrictions.
This is a problem that has symmetry.
We have even functions and odd functions.
And for the even functions, d psi dx is equal to 0.
And for the odd functions, psi of 0 is equal to 0.
OK.
So this is something that-- you choose the simplest problem.
And you use symmetry.
And bang, all of a sudden, you get fantastic insights.
So let's look at what happens to the even functions.
So let's just draw a picture of the harmonic oscillator energy
levels.
And we have a barrier, which we say maybe goes that high.
And so we have 1.
And we have 3.
And we have 5.
They're basically not affected by the barrier.
Because they have a node at the barrier.
And then we have v equals 0.
What happens to v equals 0?
Well, it hits this barrier.
And it's got a large amplitude.
And it can't accrue more phase as you go through the barrier.
So when it hits the other turning point,
it doesn't satisfy the boundary conditions.
It'll go to infinity at x equals positive infinity.
So it has to be shifted so that the boundary conditions
at the turning points are met.
And the only way that can happen is
it gets shifted up in energy a lot.
So v equals 0 is here.
Now, it can't be shifted above v equals 1.
Because that would violate the node rule.
And if you draw a picture of the wave function for v
equals 0 in the boundary region, the wave function
has to look something-- well, it has
to look something like that.
So we have two lobes.
And it's trying to make a node, but it can't.
It's a decreasing exponential.
I mean, if you have a wave going into this region
of the barrier, you can have an increasing exponential
or a decreasing exponential.
You can never satisfy continuity of the wave function
with the increasing exponential.
But you can with the decreasing exponential.
And so the height of the barrier determines how close this guy
comes to having a node.
It never will.
And how does this compare to the wave function for v equals 1?
Well, the wave function for v equals 1 looks like this.
The amplitude in this lobe and the amplitude in that lobe
are the same.
But the sign is reversed.
And so basically, this picture tells you
that these two levels have almost exactly the same energy.
So v equals 0 is shifted up.
v equals 2 is shifted up, but not quite so much.
And v 4 is shifted up hardly at all.
And so you get what's called level staggering.
And this level staggering is the signature of tunneling.
This is how we know about tunneling, the only way we
know about tunneling.
So we measure the energy levels.
And it tells us how are the wave functions sampling
this barrier.
Now, this is a childish barrier.
And there is a real barrier--
molecules isomerize.
And they isomerize over a barrier.
And the barrier isn't necessarily at x equals 0.
But if you understand this problem,
you can deal with isomerization.
Now, I'm an author of a paper that's
just appearing in Science in the next few weeks
on the isomerization from vinylidene to acetylene.
There's a barrier involved.
So these sorts of pictures are important for understanding
those sorts of phenomena.
Now, so I'm done really.
So what we are now encountering with the time
dependent Schrodinger equation is discovering
how dynamics, like tunneling, is encoded
in an eigenstate spectrum.
Because the encoding is level staggering eigenstates.
So people normally have this naive idea
that eigenstate time independent Hamiltonian spectroscopy
does not sample dynamics because it's only
measuring energy levels.
Real dynamical processes are time dependent.
But the dynamics is encoded in energy level patterns.
And that is actually my signature
in experimental spectroscopy.
I've looked for ways in which dynamics is
encoded in eigenstate spectra.
And chemists are interested in dynamics much more than
in structure.
So that's it for today.
I will see you on Wednesday.