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D— x(t) = b— x(t), t
and w— by
dx(t) = b— x(t), t dt + dw— (t).

85
86 CHAPTER 13

‚ +1.
Let f be a smooth function on Then
f x(t + ∆t), t + ∆t ’ f x(t), t =
‚f
x(t), t ∆t + [x(t + ∆t) ’ x(t)] · f x(t), t
‚t
‚2f
1
[xi (t + ∆t) ’ xi (t)][xj (t + ∆t) ’ xj (t)] i j x(t), t
+
2 i,j ‚x ‚x
+ o(t),
so that

+b·
Df x(t), t = ( + ν∆)f x(t), t . (13.1)
‚t
Let ν— be the di¬usion coe¬cient of w— . (A priori, ν— might depends on
x and t, but we shall see shortly that ν— = ν.) Similarly, we ¬nd

+ b— · ’ ν— ∆ f x(t), t .
D— f x(t), t = (13.2)
‚t
If f and g have compact support in time, then Theorem 11.12 shows
that
∞ ∞
EDf x(t), t · g x(t), t dt = ’ Ef x(t), t D— g x(t), t dt;
’∞ ’∞

that is,


+ b · + ν∆ f (x, t) · g(x, t)ρ(x, t) dxdt =
‚ ‚t
’∞


’ + b— · ’ ν— ∆ g(x, t) · ρ(x, t) dxdt.
f (x, t)
‚ ‚t
’∞

For A a partial di¬erential operator, let A† be its (Lagrange) adjoint with
respect to Lebesgue measure on ‚ +1 and let A— be its adjoint with respect
to ρ times Lebesgue measure. Then (Af )gρ is equal to both f A† (gρ)
and f (A— g)ρ, so that
A— = ρ’1 A† ρ.
Now

‚ ‚
+b· =’ ’b· ’ div b + ν∆,
+ ν∆
‚t ‚t
KINEMATICS OF MARKOVIAN MOTION 87

so that

‚ ‚
ρ’1 ρg = ρ’1 ’ ’b· ’ div b + ν∆ (ρg) =
+ b· + ν∆
‚t ‚t
‚g ‚ρ
’ ρ’1 g ’ b · g ’ ρ’1 b · (grad ρ)g ’ (div b)g

‚t ‚t
’1
+ ρ ν (∆ρ)g + 2 grad ρ · grad g + ρ∆g .

Recall the Fokker-Planck equation
‚ρ
= ’ div(bρ) + ν∆ρ. (13.3)
‚t
Using this we ¬nd
‚ρ div(bρ) ∆ρ grad ρ ∆ρ
’ρ’1 ’ν = div b + b · ’ν
= ,
‚t ρ ρ ρ ρ
so we get
‚ ‚ grad ρ
’ ’ b— · + ν— ∆ = ’ ’b· ·
+ 2ν + ν∆.
‚t ‚t ρ
Therefore, ν— = ν and b— = b ’ 2ν(grad ρ)/ρ. If we make the de¬nition
b ’ b—
u= ,
2
we have
grad ρ
u=ν .
ρ
We call u the osmotic velocity cf. Chapter 4, Eq. (6) .
There is also a Fokker-Planck equation for time reversed:
‚ρ
= ’ div(b— ρ) ’ ν∆ρ. (13.4)
‚t
If we de¬ne
b + b—
v= ,
2
we have the equation of continuity
‚ρ
= ’ div(vρ),
‚t
88 CHAPTER 13

obtained by averaging (13.3) and (13.4). We call v the current velocity.
Now
grad ρ
u=ν = ν grad log ρ.
ρ
Therefore,
‚ρ
‚u ‚
=ν grad log ρ = ν grad ‚t =
‚t ‚t ρ
’ div(vρ) grad ρ
= ’ν grad div v + v ·
ν grad =
ρ ρ
’ ν grad div v ’ grad v · u.

That is,
‚u
= ’ν grad div v ’ grad v · u. (13.5)
‚t
Finally, from (13.1) and (13.2),


b— x(t), t + b ·
Db— x(t), t = b— x(t), t + ν∆b— x(t), t ,
‚t

D— b x(t), t = b x(t), t + b— · b x(t), t ’ ν∆b x(t), t ,
‚t
so that the mean acceleration as de¬ned in Chapter 11, Eq. (11.15) is
given by a x(t), t where

b ’ b—
‚ b + b— 1 1
+ b· b— + b— · b ’ ν∆
a= .
‚t 2 2 2 2

That is,
‚v
=a+u· u’v· v + ν∆u. (13.6)
‚t
Chapter 14

Remarks on quantum
mechanics

In discussing physical theories of Brownian motion we have seen that
physics has interesting ideas and problems to contribute to probability
theory. Probabilities also play a fundamental rˆle in quantum mechanics,
o
but the notion of probability enters in a new way that is foreign both
to classical mechanics and to mathematical probability theory. A mathe-
matician interested in probability theory should become familiar with the
peculiar concept of probability in quantum mechanics.
We shall discuss quantum mechanics from the point of view of the rˆle o
of probabilistic concepts in it, limiting ourselves to the non-relativistic
quantum mechanics of systems of ¬nitely many degrees of freedom. This
theory was discovered in 1925“1926. Its principal features were estab-
lished quickly, and it has changed very little in the last forty years.
Quantum mechanics originated in an attempt to solve two puzzles:
the discrete atomic spectra and the dual wave-particle nature of matter
and radiation. Spectroscopic data were interpreted as being evidence for
the fact that atoms are mechanical systems that can exist in stationary
states only for a certain discrete set of energies.
There have been many discussions of the two-slit thought experiment
illustrating the dual nature of matter; e.g., [28, §12] and [29, Ch. 1].
Here we merely recall the bare facts: A particle issues from — in the
¬gure, passes through the doubly-slitted screen in the middle, and hits
the screen on the right, where its position is recorded. Particle arrivals
are sharply localized indivisible events, but despite this the probability of
arrival shows a complicated di¬raction pattern typical of wave motion. If

89
90 CHAPTER 14

one of the holes is closed, there is no interference pattern. If an observa-
tion is made (using strong light of short wave length) to see which of the
two slits the particle went through, there is again no interference pattern.




Figure 3


The founders of quantum mechanics can be divided into two groups:
the reactionaries (Planck, Einstein, de Broglie, Schr¨dinger) and the radi-
o
cals (Bohr, Heisenberg, Born, Jordan, Dirac). Correspondingly, quantum
mechanics was discovered in two apparently di¬erent forms: wave me-
chanics and matrix mechanics. (Heisenberg™s original term was “quan-
tum mechanics,” and “matrix mechanics” is used when one wishes to
distinguish it from Schr¨dinger™s wave mechanics.)
o
In 1900 Planck introduced the quantum of action h and in 1905 Ein-
stein postulated particles of light with energy E = hν (ν the frequency).
We give no details as we shall not discuss radiation. In 1924, while a
graduate student at the Sorbonne, Louis de Broglie put the two formulas
E = mc2 and E = hν together and invented matter waves. The wave
nature of matter received experimental con¬rmation in the Davisson-
Germer electron di¬raction experiment of 1927, and theoretical support
by the work of Schr¨dinger in 1926. De Broglie™s thesis committee in-
o
cluded Perrin, Langevin, and Elie Cartan. Perhaps Einstein heard of de
REMARKS ON QUANTUM MECHANICS 91

Broglie™s work from Langevin. In any case, Einstein told Born, “Read it;
even though it looks crazy it™s solid,” and he published comments on de
Broglie™s work which Schr¨dinger read.
o
Suppose, with Schr¨dinger, that we have a particle (say an electron)
o
of mass m in a potential V . Here V is a real function on ‚3 representing
the potential energy. Schr¨dinger attempted to describe the motion of
o
the electron by means of a quantity ψ subject to a wave equation. He
was led to the hypothesis that a stationary state vibrates according to
the equation

h2
¯
∆ψ + (E ’ V )ψ = 0, (14.1)
2m

where h is Planck™s constant h divided by 2π, and E (with the dimensions
¯
of energy) plays the rˆle of an eigenvalue.
o
This equation is similar to the wave equation for a vibrating elastic
¬‚uid contained in a given enclosure, except that V is not a constant.
Schr¨dinger was struck by another di¬erence [30, p. 12]:
o
“A simpli¬cation in the problem of the ˜mechanical™ waves (as com-
pared with the ¬‚uid problem) consists in the absence of boundary con-
ditions. I thought the latter simpli¬cation fatal when I ¬rst attacked
these questions. Being insu¬ciently versed in mathematics, I could not
imagine how proper vibration frequencies could appear without boundary
conditions.”
Despite these misgivings, Schr¨dinger found the eigenvalues and eigen-
o
functions of (14.1) for the case of the hydrogen atom, V = ’e/r where
e is the charge of the electron (and ’e is the charge of the nucleus) and
r2 = x2 + y 2 + z 2 . The eigenvalues corresponded precisely to the known
discrete energy levels of the hydrogen atom.
This initial triumph, in which discrete energy levels appeared for the
¬rst time in a natural way, was quickly followed by many others. Be-
fore the year of 1926 was out, Schr¨dinger reprinted six papers on wave
o
mechanics in book form [30]. A young lady friend remarked to him (see
the preface to [30]): “When you began this work you had no idea that
anything so clever would come out of it, had you?” With this remark
Schr¨dinger “wholeheartedly agreed (with due quali¬cation of the ¬‚atter-
o
ing adjective).”
Shortly before Schr¨dinger made his discovery, the matrix mechanics
o
of Heisenberg appeared. In this theory one constructs six in¬nite matrices

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