Network Theory (Part 13)

Unlike some recent posts, this will be very short. I merely want to show you the quantum and stochastic versions of Noether’s theorem, side by side.

Having made my sacrificial offering to the math gods last time by explaining how everything generalizes when we replace our finite set $X$ of states by an infinite set or an even more general measure space, I’ll now relax and state Noether’s theorem only for a finite set. If you’re the sort of person who finds that unsatisfactory, you can do the generalization yourself.

Two versions of Noether’s theorem

Let me write the quantum and stochastic Noether’s theorem so they look almost the same:

Theorem. Let $X$ be a finite set. Suppose $H$ is a self-adjoint operator on $L^2(X)$ , and let $O$ be an observable. Then

$[O,H] = 0$

if and only if for all states $\psi(t)$ obeying Schrödinger’s equation

$\displaystyle{ \frac{d}{d t} \psi(t) = -i H \psi(t) }$

the expected value of $O$ in the state $\psi(t)$ does not change with $t.$

Theorem. Let $X$ be a finite set. Suppose $H$ is an infinitesimal stochastic operator on $L^1(X)$ , and let $O$ be an observable. Then

$[O,H] =0$

if and only if for all states $\psi(t)$ obeying the master equation

$\displaystyle{ \frac{d}{d t} \psi(t) = H \psi(t) }$

the expected values of $O$ and $O^2$ in the state $\psi(t)$ do not change with $t.$

This makes the big difference stick out like a sore thumb: in the quantum version we only need the expected value of $O$ , while in the stochastic version we need the expected values of $O$ and $O^2$ !

Brendan Fong proved the stochastic version of Noether’s theorem in Part 11. Now let’s do the quantum version.

Proof of the quantum version

My statement of the quantum version was silly in a couple of ways. First, I spoke of the Hilbert space $L^2(X)$ for a finite set $X$ , but any finite-dimensional Hilbert space will do equally well. Second, I spoke of the “self-adjoint operator” $H$ and the “observable” $O$ , but in quantum mechanics an observable is the same thing as a self-adjoint operator!

Why did I talk in such a silly way? Because I was attempting to emphasize the similarity between quantum mechanics and stochastic mechanics. But they’re somewhat different. For example, in stochastic mechanics we have two very different concepts: infinitesimal stochastic operators, which generate symmetries, and functions on our set $X,$ which are observables. But in quantum mechanics something wonderful happens: self-adjoint operators both generate symmetries and are observables! So, my attempt was a bit strained.

Let me state and prove a less silly quantum version of Noether’s theorem, which implies the one above:

Theorem. Suppose $H$ and $O$ are self-adjoint operators on a finite-dimensional Hilbert space. Then

$[O,H] = 0$

if and only if for all states $\psi(t)$ obeying Schrödinger’s equation

$\displaystyle{ \frac{d}{d t} \psi(t) = -i H \psi(t) }$

the expected value of $O$ in the state $\psi(t)$ does not change with $t$ :

$\displaystyle{ \frac{d}{d t} \langle \psi(t), O \psi(t) \rangle = 0 }$

Proof. The trick is to compute the time derivative I just wrote down. Using Schrödinger’s equation, the product rule, and the fact that $H$ is self-adjoint we get:

$\begin{array}{ccl} \displaystyle{ \frac{d}{d t} \langle \psi(t), O \psi(t) \rangle } &=& \langle -i H \psi(t) , O \psi(t) \rangle + \langle \psi(t) , O (- i H \psi(t)) \rangle \\ \\ &=& i \langle \psi(t) , H O \psi(t) \rangle -i \langle \psi(t) , O H \psi(t)) \rangle \\ \\ &=& - i \langle \psi(t), [O,H] \psi(t) \rangle \end{array}$

So, if $[O,H] = 0$ , clearly the above time derivative vanishes. Conversely, if this time derivative vanishes for all states $\psi(t)$ obeying Schrödinger’s equation, we know

$\langle \psi, [O,H] \psi \rangle = 0$

for all states $\psi$ and thus all vectors in our Hilbert space. Does this imply $[O,H] = 0$ ? Yes, because $i$ times a commutator of a self-adjoint operators is self-adjoint, and for any self-adjoint operator $A$ we have

$\forall \psi \; \; \langle \psi, A \psi \rangle = 0 \qquad \Rightarrow \qquad A = 0$

This is a well-known fact whose proof goes like this. Assume $\langle \psi, A \psi \rangle = 0$ for all $\psi.$ Then to show $A = 0,$ it is enough to show $\langle \phi, A \psi \rangle = 0$ for all $\phi$ and $\psi$ . But we have a marvelous identity:

$\begin{array}{ccl} \langle \phi, A \psi \rangle &=& \frac{1}{4} \left( \langle \phi + \psi, \, A (\phi + \psi) \rangle \; - \; \langle \psi - \phi, \, A (\psi - \phi) \rangle \right. \\ && \left. +i \langle \psi + i \phi, \, A (\psi + i \phi) \rangle \; - \; i\langle \psi - i \phi, \, A (\psi - i \phi) \rangle \right) \end{array}$

and all four terms on the right vanish by our assumption. █

The marvelous identity up there is called the polarization identity. In plain English, it says: if you know the diagonal entries of a self-adjoint matrix in every basis, you can figure out all the entries of that matrix in every basis.

Why is it called the ‘polarization identity’? I think because it shows up in optics, in the study of polarized light.

Comparison

In both the quantum and stochastic cases, the time derivative of the expected value of an observable $O$ is expressed in terms of its commutator with the Hamiltonian. In the quantum case we have

$\displaystyle{ \frac{d}{d t} \langle \psi(t), O \psi(t) \rangle = - i \langle \psi(t), [O,H] \psi(t) \rangle }$

and for the right side to always vanish, we need $[O,H] = 0$ latex , thanks to the polarization identity. In the stochastic case, a perfectly analogous equation holds:

$\displaystyle{ \frac{d}{d t} \int O \psi(t) = \int [O,H] \psi(t) }$

but now the right side can always vanish even without $[O,H] = 0.$ We saw a counterexample in Part 11. There is nothing like the polarization identity to save us! To get $[O,H] = 0$ we need a supplementary hypothesis, for example the vanishing of

$\displaystyle{ \frac{d}{d t} \int O^2 \psi(t) }$

Okay! Starting next time we’ll change gears and look at some more examples of stochastic Petri nets and Markov processes, including some from chemistry. After some more of that, I’ll move on to networks of other sorts. There’s a really big picture here, and I’m afraid I’ve been getting caught up in the details of a tiny corner.

This entry was posted on Tuesday, October 11th, 2011 at 5:20 am and is filed under mathematics, networks, physics, probability. You can follow any responses to this entry through the RSS 2.0 feed. You can leave a response, or trackback from your own site.

6 Responses to Network Theory (Part 13)

Bossavit says:

11 October, 2011 at 1:14 pm

Why is it called the ‘polarization identity’? I think because it shows up in optics, in the study of polarized light.

I always assumed it came from geometry, namely the concept of reciprocal polar: something like, if (Ax, x) = 1 is the equation a quadric, the polar form (Ax, y) gives the polar of point x as the hyperplane {y : (Ax, y) = 1}, etc. Could you give more hints about the “optics” thing? (I can well imagine a connection, but what about the historical order? Studies in optics by, say Fresnel, etc., leading to the concept of polarity in geometry, or the other way round?)

Thanks for the very clear current series of posts.

A.B.

Reply
- John Baez says:
  
  12 October, 2011 at 3:16 am
  
  Bossavit wrote:
  
  Could you give more hints about the “optics” thing?
  
  Unfortunately I’m having no luck remembering or finding what I once read about this. The best I can do now is the abstract of this paper:
  
  • W. D. Montgomery, Phase retrieval and the polarization identity, Optics Letters 2 (178), 120-121.
  
  Abstract: A mathematical identity allows us to express the product of two complex light fields as a sum of the intensities of four different superpositions of the two. One common holographic scheme and one proposed by Gabor and Goss turn out to be the experimental realizations of the first term and the sum of the first two terms respectively of this identity. One scheme that we propose, using the identity, bears a strong resemblance to a proposal of Wiener for producing an operational equivalent of a nonlinear transducer.
  
  Of course this doesn’t prove the name polarization identity came from the study of polarized light, but it fits the story I once heard.
  
  (I haven’t bothered to read the article because it’s not freely available, so I’d need to do a little work to access it through my university library. But it could give extra clues.)
  
  Thanks for the very clear current series of posts.
  
  You’re welcome! I’m having fun writing them, but it’s always more fun when I hear that people are still reading them.
  
  Reply
Jon Rowlands says:

11 October, 2011 at 3:16 pm

Typo: $L^1$ and $L^2$ are interchanged in “Two versions of ..”.

Reply
- John Baez says:
  
  12 October, 2011 at 2:25 am
  
  Thanks very much – I’ll fix that!
  
  By the way, on this blog – or I believe any WordPress blog – you need to write
  
  $latex L^1 $
  
  to get TeX to work – the “latex” must appear directly after the first dollar sign, without a space. If you do that, you’ll get
  
  $L^1$
  
  Reply
Arjun Jain says:

27 June, 2013 at 3:00 am

You say that for any self-adjoint operator $A$ we have,
$\forall \psi \; \; \langle \psi, A \psi \rangle = 0 \qquad \Rightarrow \qquad A = 0$ , but in the proof, where are you using the fact that $A$ is self adjoint?

Reply
- John Baez says:
  
  27 June, 2013 at 8:34 am
  
  I was proving that if
  
  $\displaystyle{ \frac{d}{dt} \langle \psi(t), O \psi(t) \rangle = 0}$
  
  for all states $\psi(t)$ obeying Schrödinger’s equation
  
  $\displaystyle{ \frac{d}{dt} \psi(t) = -i H \psi(t) }$
  
  then
  
  $[O,H] = 0$
  
  This is true if $O$ and $H$ are self-adjoint, but not necessarily otherwise. The argument goes like this:
  
  If this time derivative vanishes for all states $\psi(t)$ obeying Schrödinger’s equation, we know
  
  $\langle \psi, [O,H] \psi \rangle = 0$
  
  for all states $\psi$ and thus all vectors in our Hilbert space. Does this imply $[O,H] = 0$ ? Yes, if $O$ and $H$ are self-adjoint, because i times a commutator of a self-adjoint operators is self-adjoint, and for any self-adjoint operator $A$ we have
  
  $\forall \psi \; \; \langle \psi, A \psi \rangle = 0 \qquad \Rightarrow \qquad A = 0$
  
  Reply

You can use HTML in your comments. You can also use LaTeX, like this: $latex E = m c^2 $. The word 'latex' comes right after the first dollar sign, with a space after it. Cancel reply

Enter your comment here...

Fill in your details below or click an icon to log in:

Email (required) (Address never made public)

Name (required)

Website

You are commenting using your WordPress.com account. ( Log Out / Change )

You are commenting using your Twitter account. ( Log Out / Change )

You are commenting using your Facebook account. ( Log Out / Change )

You are commenting using your Google+ account. ( Log Out / Change )

Cancel

Connecting to %s

	John Baez on Markov Models of Social Change…
	John Baez on Markov Models of Social Change…
	Vanessa Schweizer on Markov Models of Social Change…
	Vanessa Schweizer on Markov Models of Social Change…
	John Baez on Markov Models of Social Change…
	nad on Markov Models of Social Change…
	Metamorf on Markov Models of Social Change…
	John Baez on Network Theory I
	John Baez on Markov Models of Social Change…
	Vanessa Schweizer on Markov Models of Social Change…

Azimuth