adiabatic motion in classical physicspeople.roma2.infn.it/~cini/ts2016/ts2016-11.pdffrom griffiths...
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1
Adiabatic motion in classical Physics
From Griffiths Introduction to Quantum Mechanics
Key concept: the pendulum will keep swinging regularly parallel to the same planeif external condition change little during an oscillation. In Quantum Mechanics the Born-Oppenheimer approximation is somewhat similar.
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222
Adiabatic theorem (Kato 1949)
Hamiltonian depends on
R=set of
parameters
slow
At 0 system in eigenstate, but R=R(t) adiabatically in (0,T), Tt
( ) [ ( )] ( )
( 0) [ (0)]
n n
n n
i t H R t ttt a R
Formal expansion over instantaneous complete set
of eigenstates of [ ( )] treated as static:
( ) ( ) [ ( )] ( ) [ ( )]
(0) 1
n n n m mm n
n
H R t
t c t a R t c t a R t
c
Basic for perturbation theory, Berry phase etc
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Adiabatic theorem:
Let [ ] have discrete spectrum with no degeneracy
For slow enough changes
[ ] [ ] [ ] [ ]
0 for in adiabatic limit.n n n
m
H R
H R a R E R a R
c m n
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Adiabatic Theorem (see Griffiths, Meccanica Quantistica)
Time-dependent part of
'( ) ( )
H
H t Vf t
Initial state ( 0) i
n nt
'( )
final Hamiltonian stationary states
( )
f
m
f f f
m m m
H V
H V E Assumptions:T very long,f(t) gradual,
discrete spectrum, no level crossing
Temporary assumption: for the moment
assume V very small, too
Thisenables first-order time-independent
perturbation theory for stationary states
final
f kmm m k
k m m k
V
E E
f(t)
tT0
1
4
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5
For t=0 system in level n: initial state ( 0) .
Use perturbation theory,too,time-
to evaluate ( ) in termsof the initial eigenstates.
( ) ( ) ( ) where ( ) (0) .
Recalli
depen
ng
dent
tim
m
i
n n
E ti
m m m lm
t
T
t c t t t e
( ) '
n 0
0
e-dependent part of : '( ) ( )
mplitude of n , .
mplitude of remaining in initial state:
n n ( )
( ) ' ( ')
1 ' ( ')
m nE E tt i
m
t
nn
m
n
H H t Vf t
A m l n
A
ic t V dt
ic
f
t V dt f
t
t e
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( ) '
( ) '
n 0
( ) '
ln 0
( ) '
mplitude of n , .
Insert identit
( ) ' ( '
y :
)
( ) ' ( '
'
)'
m
n
m
m
n
n
n
mE E t E E ti
E E tt i
m m
E E tt i
m
m n
i
m n
ic t V dt f t e
i i dc t V dt f t e
E
A m l n
i de
d
E E
E
edt
t
Trick to exploit the smallness of
( ) ( ) '
ln
0by parts ( ) ( ) ' ( ')
'
l n l nE E t E E ti t i
l
l n
V dc t f t e dt e f t
E E dt
( )
n
0
In adiabatic case, ( ) ( ) , for m ,
while ( ) 1 ' ( ').
m nE E ti
mm
m n
t
n nn
Vc t f t e n
E E
ic t V dt f t
( )df t
dt
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ln
n 0
Amplitude to jump to state , approximated here in first order,
( ) by time-depenent p.t. by time-indepenent p.
(1 ' ( '
t.
))[ ]n
f
m
Et
Ti
kmn l m k
l n k ml m k
n
n
iV dt
m n
T
VVe
E E E Ef t
Now obtain the transition amplitude in 1st order:
take 1 ( ) and (right) :
This contributes .n
kmk
m k
E Ti
nm
m n
n m
Vleft
E E
Ve
E E
lnNow, take (left) and (right) : :
This contributes .
n n
n
E T E Ti i
nml m n
l n l n m n
E Ti
nm
m n
VVe e
E E E E
Ve
E Enet result: 0
No transitions in first order. This is the Kato theorem.
Now we remove restriction to small V
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f(t)
tT0
1
Divide (0,T) in N time
slices
In every slice,
VV
N
Since first-order is 0,
total goes like
2
20
VN for NN
Adiabatic theorem:
no degeneracy
for sl
[ ] discrete spectrum with
[ ] [ ] [ ] [ ]
0 for in adiabatic li
ow enough chang
m
es
it.n n n
m
H R
H R a R E R a R
c m n
The adiabatic theorem grants that the system remains in state n, but does not
specify what happens to the phase.
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Density operator
ˆOne introduces the density operator when the system
in a mixed state has probability p of being in state .
ˆ ˆ ( )
Density matrix is the matrix of
n
n
n
i i i i i
i
p n n
n
A p A A Tr A
ˆ in any basis.
exp( )In equilibrium, p on the basis of H eigenvectors.n
n
E
Z
If a system is known to be in quantum state the expectation value
of any operator A is .
If a system is in an and is known to be in quantum sti ate
with probabili
mpure or mixed st
p
te
t
a
y
i
i i
i
i
A
the expectation value of any operator A is
.i i i
i
A p A
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ˆLet T=0 (absolute 0) and 0 0
(system in instantaneous ground state at time 0).
ˆIf evolution is adiabatic 0 0 all the time ( theorem).
is
Kato
Now assume that the system evolves slowly, but at a finite speed.
One must envisage an adiabatic perturbation theory to evaluate the
corrections to the exactly adiabatic limit. Corrections are particularly
important to evaluate matrix elements that vanish in the ground state.
Adiabatic perturbation theory
Quasi-adiabatic density matrix (Niu-Thouless)
Slow t dependenc
ˆ 0,
e
with small by adiabatic theor
0, instantaneous density operat
e
or:
mi
it t
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111111
00
Slow t dependence
with small by adiabatic theorem:
with m and n excited on instantaneous
e
First-order
igenstate basis is twice small negligible i
cor
f 0,
0, , , 0rectio
0
n
.
on
i
m
nn
n
m
t n t n t
n
,t
0
0
0 changes slowly.
We shall find that the off-diagonal density matrix is
0
which is almost self-
evident on dimensional gro d
un s.
n
n
niE E
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121212
[ , ] Slow t dependence , with
( ) [ , ]
small by adiabatic the
0, 0, instantaneous density matrix a
orem negligible
get
t T=
from equation of motion ( [
0
) ,
i i
i
i i
i i
di Hdt
t
di Hdt
didtdi Hdt
t
] .
et's take matrix element 0
0 ( 0, 0, ) 0 [ , ]
L n
di t t n H ndt
0( ) 0, ( ) 0, [ , ( )] 0, 0, 0, 0, 0
( 0, 0, ) [ , ]
iH t t E t t H t t t H H t t
di t t Hdt
Proof
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131313
0
0
0
0
0 0 [ , ] ( )( 0, 0, )
( 0, 0, )0 ( 0, 0,
0
()
)
n n
n
n
dt t
dtd
i n H n E
n
E E
t tddt t t
E
n ndt
i eeded
0, , 0,
acts on bra and ket:
( 0, 0, ) 0,0 0
b
0,( ) ( ), 0, 0, 0,
0ut , 0, 1
t
d
dt
d d dt t t t t t
dt dt dt
t tt
n n n
t n
tt
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0 ( ) , but since
one can simplify:
( 0, 0, ) 0,
( 0, 0, ) 0,
0, , 0,
) 0, ,0 ( ( )
d dt t t
dt dt
d
n n t
n nd
t t t t n td
n t
tt
t
dt
0
0
0n
n
niE E
0 0 0
0
ˆThe correction to the expectation value of any operayor A
)0
(n n n
n n n
A Tr A t An
iE E
A14
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1515
Quantum phases
Gauge Transformations
Without the gauge invariance, any theory is untenable. In classical theory,the Hamiltonian of a charged particle is
2( )( )
2
ep AcH eV xm
where p is the canonical momentum and A the vector potential. Both are unobservable.The SE reads:
2( ){ ( )}
2
ep Ac eV x im t
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1616
1' ( , ) 'A A x t V V
c t
2( [ ])1 '
{ [ ( ) ]} '2
ep Ac e V x im c t t
This gives a new Schroedinger equation and a new wave function:
;One could have started with new potentials giving the same fields:
which is solved by
( , )Ψ'(x,t)=Ψ(x, )exp[ ]; nochange in the physics.
ie x tt
c
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1717
Galileo Transformations
2 2 2 2
Let system K' move with speed w with respect to K: for a particle
r=r'+wt
1 1 1 1p=p'+mw E= (w v') w v' wv' ' w wv'
2 2 2 2m m m m E m m
Plane wave in K =exp[ pr-Et]
Plane wave in K' ' =exp[ p'r'-E't]
i
i
2
2
Plane wave in K
1 ( )=exp[ (p'+mw)(r'+wt)-( ' w wv')t]
2'
= '( ') exp[ mw ] . Setting r'=r-wt2
= '( ') exp[ (mw )] 2
ir E m m
i r rr
i mw tr r
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1818
2 ( , ) { ( )} ( , ) ;
2in a moving frame
' , ' , ' .
p x teV x x t i
m t
x x vt y y z z
( , , , )
2
'( ', ', ', ) ( , , , )
( , , , )2
i x y z tx y z t x y z t e
mwr mw tx y z t
2
( )= '( ') exp[ (mw )] 2
holds for all Fourier components.
i mw tr r r
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1919
Superconductor Thin insulatorSuperconductor
R
emf
Macroscopic quantum phenomena: Josephson effect
2* * 2
*
Ginzburg-Landau: order parameter with charge
[ ] | | 02
=2e
S
e
e eJ A A
mi m c
1
1 1| |ie 2
2 2| |ie
( )
1 2
1 2
* *
1 2 1 2 2 1
Matching ( ) in barrier ( ) , barrier width
and approximately constant
sin .
A phase difference across the barrier implies a current with no bias (DC josephson e
z z b
S
z z e e b
J
ffect)
In elementary quantum problems if there is no bias, ( ) can be taken real and there is no current.
In ordinary circumstances, there is dissipation and no phase coherence over
macroscopic distan
z
ces. But superconductivity is a macroscopic quantum
phenomenon.
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AC response to DC bias !
0 0 0
2sin ( ) , constant
eVI I t t I
2
1
2 1
1 A bias which creates a energy difference proportional to t
analogous t
o to th
AC josephso
e e factor o
n effect
f elementary QM,
E
e
im
iEt
SJ
eVt
* *
2 1
0 0
2 2 1si
2sin (
n
) ,eV
I I t t
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Topologic phases
Start from north pole towards Rome bringing a pendulum oscillating parallel
to the Rome meridian, reach the equator, then turn left along the equator
without changing the plane of oscillator, reach the Parallel of Moscou and
follow it bach to the North pole; now the oscillator swings towards Moscou.
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2222
22
Topologic phasesPancharatnam phase
The Indian physicist S. Pancharatnam in 1956 introduced the concept of a geometrical phase.
Let H(ξ ) be an Hamiltonian which depends from some parameters, represented by ξ ; let |ψ(ξ )> be the ground state.
Compute the phase difference Δϕij between |ψ(ξ i)> and |ψ(ξj)>
However, this is gauge dependent and cannot have any physical meaning.Now consider 3 points ξ and compute the total phase γ in a closed circuitξ1 → ξ2 → ξ3 → ξ1; remarkably,γ = Δϕ12 + Δϕ23 + Δϕ31
is gauge independent!
Indeed, the phase of any ψ can be changed at will by a gauge transformation, but such arbitrary changes cancel out in computing γ. This clearly holds for any closed circuit with any number of ξ. Therefore γ is entitled to have physical meaning.
There may be observables that are not given by Hermitean operators.
We may define .iji
i j i je
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2323
In the case of H2 this can be gauged away, but with three or more atoms the physical meaning is that a magnetic flux φ is concatenated with the molecule; changing φ by a fluxon has no physicalmeaning, however.
b
7 2
h h 0a0
Peierls prescription: to introduce A
2 it t exp[ A.dr], 4 10 Gauss cm fluxon
hc
e
For instance, consider a Linear Combination of Atomic Orbitals (LCAO) model fora molecule or cluster (or a Hubbard Model, neglecting overlaps)
By complex
hoppings, one
can introduce a
concatenated
magnetic flux
23
A.dr
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2424
3-site cluster with flux
( )gs gsE E
23 13 12
0
1, ,
2
ie
e
c
1
2
3
Ground state Energy Egs() has period=2
In[12]:= h :
0 EI 1
E I 0 1
1 1 0
;
ListPlot Table , Min Eigenvalues h , , 0, 6 , .1 ,
PlotJoined True, AxesLabel , E ,
Ticks 0, Pi, 2 Pi, 3 Pi, 4 Pi, 5 Pi , 0, 1
Out[12]=
2 3 4 5
Egs
0
hc
e
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25
Adiabatic theorem and Berry phase
( ) ( )2
0
| ( ) | 1 ( ) , where along with
( ) ' [ ( ')] expected dynamical phase,
there is also the topological Berry phase .
n ni t i t
n n
t
n n
c t c t e
t dt E R t
Let [ ( )] depend on a set of several parameters
which vary in time.
Consider the evolution of n-th eigenvector
starting from t=0. Expanding on an
instantaneous eigenvector basis,
( ) ( ) [
n
n n n
H H R t
t c t a R
( )] [ ( )], with (0) 1. However if the
evolution is adiabatic, we know that we can drop [ ( )].
Therefore, ( ) is enough.
m m nm n
m mm n
n
t c a R t c
c a R t
c t
25
Sir Michael Berry
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26
since (R[ ]) , one findsn R n
dRa t a
t dt
To find ( ), let us impose that .n nt i Ht
( ) ( )
0
Using the ansatz ( ) [ ( )] ,
here ( ) ' [ ( ')],
n ni t i t
n n
t
n n
t a R t e
w t dt E R t
0( ) ' [ ( ')]
( ) ( )( ) { [ ( )] }
t
n nn n
ii t dt E R t
i t i t
n n n n R n
it a R t e E i R a e
t t
( ) ( )
The r.h.s. of the Schroedinger equation reads:
( ) [ ( )] .n ni t i t
n n nH t E a R t e
( ) ( ) ( )
Therefore, the Schroedinger equation reads:
n nn ni ti t i
n n
i
nR
t
n nE ai R e E ea
( )
that is,
0n ni t i
n R ni R a e
{a }=instantaneous eigenvector basis. n
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272727
( )Result: 0n ni t i
n R ni R a e
[ ( )] [ ( )]n n R niR a R t a R t
0 0
The matrix element looks similar to a momentum average,
but the gradient is in parameter space. The overall phase
change is a line integral
. .
This has no meaning, it's a gau
T T
n n R n n R ni dt a a R i a a dR
ge, but...
( ) is a topological phase
and vanishes in simply connected parameter spaces (no holes)
but in multiply connected spaces yields a quantum number!
n n R n
C
C i a a dR
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2828
Recall:
Total H (( , ( , )) )tot NeT rH r R RT VR r set of electron coordinates
set of nuclear coordinates
r
R
2 2
2eglect ( ) . , ( , )
2
adiabatic hamiltonian for electrons. Solve , , ( ) ,
N e e
e n n n
N T R H r R T V r RM R
H r R r R E R r R
that ( , ) ( ) ( , )is, tot N eH r R T R H r R
2 2
0 2Then, use ( ) as a potential and
2NE R T
M R
2 2
02Within : one expects nuclear motion.
2BO R E R W R
M R
Vibronic coupling and the ‘unexpected’ Berry phase
Born-Oppenheimer approximation: the recipe
How good is this approximation?
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Nuclear wave Functions do not (strictly) exist
0
0 0
( , ) ( ) ( , )
( , ) electron
an
calculated with nuclei at R.
satz : trial r R R r R
r R
The Adiabatic Approximation is a cheap way to go somewhat beyond.
Adiabatic= assuming evolution confined to lowest (n=0) energy surface
computed solving for electrons at fixed R, seek (R) variationally
Nuclear wave Functions Beyond Born-Oppenheimer
There is a wave function that depends on electrons and nuclei and cannot
be factored.
Nuclei and electrons are entangled.
Even in the H atom problem there exists no nuclear wave function.
On the other hand we do need physically motivated approximations.
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0ansatz: ( , ) ( ) ( , )trial r R R r R
set of electron coordinates
set of nuclear coordinates
( ) nuclear wavefunction
r
R
R
0 0( ) ( ,[ ) ( )] ( , )tot N eF H TR RHr R R r
Variational approach to based on Energy functional
2 2
02Does yield:
2F R E R W R
M R
0 0 0( ) ( , ) ( , ) ? This would be the BOeE R r R H r Rwhere
2
02
2* * * *
0 0Minimize ( ) ( ) ( ) ( ) ( )2
drdR dR E R R R W dR R RM R
W=Lagrange multiplier (normalization)
NTeH
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we need the derivative:
2
0
2
0
2
0 2 02 22 .
Minimize:
R R RR R
* *
0
2 2*
2
2* * * *
0 0 0 0 02
( ) ( ) ( ) ( ) ( )
]2[2
drdR dR d
dR R E R R W d
dRM R
R
rR R R
R R
2
0 02
terms involving
andR R
*Vary and find best
22 2* *0 00 0
2
2
2
2
0 ( ) ( ) ( ) )
( )
( ()2
2R dr dr
M
RE R R R W RM
R R M R
R
The electron wave function
depends parametrically on
nuclear coordinates.
0 0ansatz: ( , ) ( , ) ( ) ( , )trial r R r R R r R
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200 0
nonadiabatic ( ) often ignored since for real functions
1 0
2
however this is not always the case! Not even with 0.
(see below Berry phase can arise).
R
dr drR R
B
a
22* 00 2
Moreover the excuse for neglecting the other term is:
( )*electron kinetic energy.2
Not reassuring. Typically vibrations are 0.1 eV or less, electronic jumps
require 1 eV or more.
mdr O
M R M
But close electronic levels can be mixed by vibrations!
22 2
2 2
02
* *0 00 0 2
( )2
unespected, gauge-dependent nonadiabatic term
( ) ( ) ( ) ( )2
)
!
(
R dr drM R R
E R R R W RM
M
RR
R
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Recall the Jahn-Teller
theorem:
any nonlinear molecule with a spatially degenerate electronic ground state
will undergo a geometrical distortion that removes that degeneracy.
True within the Born-Oppenheimer approximation.
Born-Oppenheimer Approximation:
Neglect of nuclear momenta
The energy surfaces have NJT several equivalent
minima corrisponding to different distortions; e.g. a cube can be squeezed in several equivalent ways.
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At strong vibronic coupling , the energysurfaces have NJT deep and distant
minima and the nuclear degrees of freedomcan hardly tunnel between them. Then, the
kinetic energy of the nuclei does not play a role, and one can observe a static JT effect with
broken symmetry.
At weak couplingthe system oscillatesbetween several
Minima and , one
speaks about dynamic JT effect ;
the overall symmetry remains unbroken.
The time scale of the experiment is the criterion for weak and strong.
In fast experiments with hard X rays the symmetry is broken
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2 2
2
Full problem : ( , ) ( ) ( , ) ( ) ( , )
( , ) ( , )( ) ,2
( , )
tot N e N e
tot toN t totT RM
H r R T R H r R T R T r V r R
H r R r R W r RR
In this more complex case we do not attempt a variational approach but we must allow the mixing of the different minima.
Several interacting Jahn-Teller minima
0 0
0
The nuclear motion is the unknown. Scheme:
compute the electronic ( , ) with fixed
corresponding to all the minima, with symmetrically distorted
geometries. Different minima yield ort
e
n n n
n
r R R
R
0hogonal ( , ), otherwise
we orthogonalize.
e
n nr R
Nuclear wave Functions Beyond Born-Oppenheimer
0
0 0
( , ) (
We must generalize to s
) ( , )
where ( , ) electron calculated with nuclei at R.
everal minima the above approach
tot
trial r R R r R
r R
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New Ansatz: summing over the minima,
( , ) ( ) ( ).n
tot e
trial k k
k
r R R r
The the electron-nuclei interaction ( , ) mixes the
orthogonal ( ) for different minima and the nuclear ( ).e
n n
V r R
r R
( , ) ( ) ( , )tot N eH r R T R T r V r R
0
*
0
Substitute ( , ) into ( , ) ( , ) ( , )
take the electronic scalar product with ( , ) and get
( ) [ ( , ) ] ( ) ( , ).
tot tot tot
tot
e
m
ne e
m tot k k
k
r R H r R r R W r R
r R
dr r H r R W R r R
*
0 0
More explicitly,
( , ) ( ) ( ) ( ,( , ) ) 0e
e e
m N k k
k
dr r R T R W R RT r r R rV
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* (( ) ( ) ( ) ( ), ) 0e e
m N k k
k
eT r V rdr T WRr R R r
2 2*
2
Use shorthand notation :
( )
( , )
( , ) ( ) ( ) 02
e
e
e e
m k k
k
H r R
H r Rdr r W R rM R
dr integrates over electrons, and we are assuming orthogonality of electronic wave functions. Upon integration over r only k=m remains and we get the simplified first term :
2 2 2 2*
2 2( ) ( ) ( ) ( ). Hence,
2 2
e e
m k k m
k
dr r R r RM R M R
2 2
*
2( ) ( ) ( ( )) (, ) 0
2m m k
k
e kH r RR dr r W R rM R
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*Set: ( ) ( ) ( , ) ( )
matrix elements of the electronic Hamiltonian between electronic
wave functions belonging to different minima.
e e
mk m e kV R dr r H r R r
22
2
( )( ) ( ) 0
2
coupled equations for the nuclear wave functions, that
mix those of different minima via the electronic .
effective nuclear dynamics accounting for the effect of
mmk mk k
k
mk
RV W R
M R
V
electrons.
2 21 11 12 1
2
2 21 22 2
Our unknown is a column vector: for 2 minima we get
( ) ( )
( ) ( )2
R V V R
R V V RM R
1 2
Our unknown is a column vector: for 2 minima we get
( ), ( ) nuclear wave functions for minima 1,2.R R
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11 1
2 2*
2
1
. . .
. . . . .
. . . . . , ( ) ( ) ( , ) ( ).2
. . . . .
. . .
n
e e
JT mk m e k
n nn
V V
H V R dr r H r R rM R
V V
Generally, the Nuclear wavefunctions are obtained from matrix
Schroedinger equation; the matrix is the Jahn-Teller Hamiltonian
2
2 must be written i terms of normal coordinates, thus excluding translations and rotations. For n=2,
R
2 2 2 2
2 2
2V(x) V(x) V(y) V(y)
V(x) V(x) V(y)2 2 V(y)
xx xy xx xy
x y
yx yy yy x yx y
JT q q KM q
HM q
q
2x2 matrices represent
operators acting on
nuclear wave functions
( , )x y
1 2The minima ( ), ( ) are linear combinations
of the normal modes of the same symmetry, thus we
analyze the effects of normal modes.
R R
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x
y
1
23
3
x y
Example of problem: Na molecule
, known electronic wave functions E
By Jahn-Teller theorem: symmetric geometry is unstable,
Electronic degeneracy challenged by degenerate vibratio
E
x y
nal mode.
, normal modes E producing potentials (V(x),V(y)) acting on electrons
and driving the nuclei to a two-state situation, reminiscent of a spin.
q q
40
vibronic couplingE
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Group theory predicts the form of the vibronic interaction, using the direct
product of representations, but here I skip the argument (see Topics and
Methods page196) leading to:
2 2 2 2
2 2
2V(x) V(x) V(y) V(y)
V(x) V(x) V(y)2 2 V(y)
xx xy xx xy
x y
yx yy yy x yx y
JT q q KM q
HM q
q
2x2 matrices represent
operators acting on
nuclear wave functions
( , )x y
2 2 2 22
2 2
0 0
0 02 2x y
y
J
x
TH q q KqM q M q
2 2 2 22 2
2 2that is, [ ] ( )
2 2JT x x y y x y
x y
H q q K q qM q M q
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2 2( , ) like (x,y)
The mode could be of this symmetry.
xy x y E
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2 2 2 22
2 2
0 0
0 02 2x y
y
J
x
TH q q KqM q M q
2 2 2 22 2
2 2that is, [ ] ( )
2 2JT x x y z x y
x y
H q q K q qM q M q
Incidentally: Second-quantized version:
† † † †1 1( ) ( ) '[( ) ( ) ]
2 2JT x x y y x x x y y yH a a a a a a a a
(two levels and two-bosons problem) and is among those exactly solved by the recursion method of Excitation Amplitudes. Here we shall consider the static limit.
x
y
1
23
2 2 2 22 2
2 2[ ] ( )
2 2JT x x y z x y
x y
H q q K q qM q M q
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Although the model can be solved, we shall work out the Born-Oppenheimer limit M :
molecule with static distortion, to obtain the JT Hamiltonian acting on nuclear coordinates
and the nuclear wave functio
2 2
ns. One can study their angular dependence
setting cos , q sin ,
0 1 1 0 0 cos sin 0.
1 0 0 1 cos 0 0 sin
xJ
y
yT
xq q q
q KH q Kq q q q
x
y
1
23
<K> q2 is an additive constant, with no dynamics, and formally HJT is the Hamiltonian for a spin in a magnetic field B = (qx, 0, qy).
specifies the mixture of x and y normal modes of lowest energy
including the vibronic coupling
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2 2:sin cos
cos si
sin cosM
cos
M
s n
n
i
JTH q Kq q Kq
2
Born-Oppenheimer limit M
0 cos sin 0
cos 0 0 sinJTH q q Kq
M has eigenvalues ±1, independent of
x
y
1
23
x y
2x2 matrices represent operators acting on nuclear
wave functions ( , ),
represents frozen (M ) nuclear displacements.
2
2
independent of
independ
1 E =
1 E
= ent o - f
JT
JT
M
M
q Kq
q Kq
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Here the potential energy surfaces E(q) are obtained by rotating two intersecting parabolas around the energy axis.
46
Minimum away from q=0. Energy eigenvalues independent of angle, but
nuclear wave function depends on angle in a special way.
q
EJT(q)
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Wizard heat singularity Multiply connected parameter space Berry phase
Modes of E symmetry of tetrahedral molecules
48
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( , ) ( , )( , )
( , ) ( , )
x y x y
JT x y
x y x y
a q q a q qH E q q
b q q b q q
Eigenvalue -1Eigenvalue +1
cos( )2 4
( )
sin( )2 4
sin( )2 4
( )
cos( )2 4
This changes sign under + 2 , which is
normal for spin rotation, but wrong here.
Nuclear wave functions must be single-valued
functions of normal coordinates!
2sin cos
cos sinJTH q Kq
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Eigenvalue -1
Eigenvalue +1
Berry phase!
We did an honest calculation. Why do we get
a wrong result?
We can fix it, but must insert
phase factors:
cos( )2 4
( )
sin( )2 4
sin( )2 4
( )
cos( )2 4
2
cos( )2 4
( )
sin( )2 4
i
e
2
sin( )2 4
( )
cos( )2 4
i
e
This compensates for the changed sign under + 2 .
Nuclear wave functions are single-valued but complex.