Quantum chaos of generic systems - Marko Robnik

Center for Applied Mathematics and Theoretical Physics
University of Maribor • Maribor • Slovenia
www.camtp.uni-mb.si
Quantum chaos of generic systems
Marko Robnik
Let’s Face Complexity
New Bridges Between Physical and Social Sciences
Como, Italy, 4-8 September 2017

COLLABORATORS
Prof.Dr. Tomaˇz Prosen, former PhD student, now at University of Ljubljana
Prof.Dr. Baowen Li, former postdoc, now at National University of Singapore
Prof.Dr. Gregor Veble, former PhD student, now chief aerodynamicist at
Joby Aviation
Dr. Gregor Vidmar, former PhD student, now at University of Ljubljana
Prof. Dr. Hans-Jürgen Stöckmann, University of Marburg, Germany
Dr. Benjamin Batistić, former PhD student, now postdoc at CAMTP
Dr. Thanos Manos, former postdoc, now postdoc at Jülich, Germany
Mr. ˇCrt Lozej, PhD student, CAMTP

CONTENTS
0. Motivation by example: Quantum billiards: Helmholtz equation
1. Introduction: Universality classes of spectral ﬂuctuations
2. Principle of Uniform Semiclassical Condensation (PUSC) of Wigner f.
3. Mixed type systems in the semiclassical limit:
3.1 Spectral statistics of regular and chaotic level sequences
3.2 Separation of regular and chaotic eigenstates
4. Quantum localization of chaotic eigenstates
5. Discussion and conclusions
6. References

Motivation by example
Two-dimensional classical billiards:
A point particle moving freely inside a two-dimensional domain
with specular reﬂection on the boundary upon the collision:
Energy (and the speed) of the particle is conserved.
A particular example of the billiard boundary shape as a model system:
Complex map: z → w, |z| = 1
w = z + λz2
,

Motivation by example
Two-dimensional quantum billiards
Helmholtz equation with Dirichlet boundary conditions
∂2
ψ
∂x2 + ∂2
ψ
∂y2 + Eψ = 0
with ψ = 0 on the boundary

Quantum chaos of generic systems - Marko Robnik

Example of mixed type system: Hydrogen atom in strong magnetic field
H =
p2
2me
−
e2
r
+
eLz
2mec
|B| +
e2
B2
8mec2
ρ2
B = magnetic field strength vector pointing in z-direction
r = x2 + y2 + z2 = spherical radius, ρ = x2 + y2 = axial radius
Lz = z-component of angular momentum = conserved quantity
Characteristic field strength: B0 =
m2
ee3
c
¯h2 = 2.35 × 109
Gauss = 2.35 × 105
Tesla
Rough qualitative criterion for global chaos: magnetic force ≈ Coulomb force
(Wunner et al 1978+; Wintgen et al 1987+; Hasegawa, R. and Wunner 1989,
Friedrich and Wintgen 1989; classical and quantum chaos: R. 1980+)

spectral unfolding procedure: transform the energy spectrum to unit mean
level spacing (or density)
After such spectral unfolding procedure we are describing the spectral statistical
properties, that is statistical properties of the eigenvalues.
Two are most important:
Level spacing distribution: P(S)
P(S)dS = Probability that a nearest level spacing S is within (S, S + dS)
E(k,L) = probability of having precisely k levels on an interval of length L
Important special case is the gap probability E(0, L) = E(L) of having no levels on
an interval of length L, and is related to the level spacing distribution:
P(S) = d2
E(S)
dS2

The Gaussian Random Matrix Theory
P({Hij})d{Hij} = probability of the matrix elements {Hij} inside the volume
element d{Hij}
We are looking for the statistical properties of the eigenvalues
A1 P({Hij}) = P(H) is invariant against the group transformations, which preserve
the structure of the matrix ensemble:
orthogonal transformations for the real symmetric matrices: GOE
unitary transformations for the complex Hermitian matrices: GUE
It follows that P(H) must be a function of the invariants of H
A2 The matrix elements are statistically independently distributed:
P(H11, . . . , HNN) = P(H11) . . . P(HNN)
It follows from these two assumptions that the distribution P(Hij) must be Gaussian:
There is no free parameter: Universality

2D GOE and GUE of random matrices:
Quite generally, for a Hermitian matrix
x y + iz
y − iz −x
with x, y, z real
the eigenvalue λ = ± x2 + y2 + z2 and level spacing
S = λ1 − λ2 = 2 x2 + y2 + z2
The level spacing distribution is
P(S) =
R3
dx dy dz gx(x)gy(y)gz(z)δ(S − 2 x2 + y2 + z2) (1)
which is equivalent to 2D GOE/GUE when gx(u) = gy(u) = gz(u) = 1
σ
√
π
exp(−u2
σ2)
and after normalization to < S >= 1
• 2D GUE P(S) = 32S2
π2 exp(−4S2
π ) Quadratic level repulsion
• 2D GOE gz(u) = δ(u) and P(S) = πS
2 exp(−πS2
4 ) Linear level repulsion
There is no free parameter: Universality

The Main Assertion of Stationary Quantum Chaos
(Casati, Valz-Gries, Guarneri 1980; Bohigas, Giannoni, Schmit 1984; Percival 1973)
(A1) If the system is classically integrable: Poissonian spectral statistics
(A2) If classically fully chaotic (ergodic): Random Matrix Theory (RMT) applies
• If there is an antiunitary symmetry, we have GOE statistics
• If there is no antiunitary symmetry, we have GUE statistics
(A3) If of the mixed type, in the deep semiclassical limit: we have no spectral
correlations: the spectrum is a statistically independent superposition of regular
and chaotic level sequences:
E(k, L) =
k1+k2+...+km=k
j=m
j=1
Ej(kj, µjL) (2)
µj= relative fraction of phase space volume = relative density of corresponding
quantum levels. j = 1 is the Poissonian, j ≥ 2 chaotic, and µ1 + µ2 + ... + µm = 1

According to our theory, for a two-component system, j = 1, 2, we have (Berry and
Robnik 1984):
E(0, S) = E1(0, µ1S)E2(0, µ2S)
Poisson (regular) component: E1(0, S) = e−S
Chaotic (irregular) component: E2(0, S) = erfc
√
πS
2 (Wigner = 2D GOE)
E(0, S) = E1(0, µ1S)E2(0, µ2S) = e−µ1S
erfc(
√
πµ2S
2 ), where µ1 + µ2 = 1.
Then P(S) = level spacing distribution = d2
E(0,S)
dS2 and we obtain:
PBR(S) = e−µ1S
exp(−
πµ2
2S2
4 )(2µ1µ2 +
πµ3
2S
2 ) + µ2
1erfc(µ2
√
πS
2 )
(Berry and Robnik 1984)
This is a one parameter family of distribution functions with normalized total
probability < 1 >= 1 and mean level spacing < S >= 1, whilst the second moment
can be expressed in the closed form and is a function of µ1.

THE IMPORTANT SEMICLASSICAL CONDITION
The semiclassical condition for the random matrix theory to apply in the chaotic
eigenstates is that the Heisenberg time tH is larger than all classical transport times
tT of the system!
The Heisenberg time of any quantum system= tH = 2π¯h
∆E = 2π¯hρ(E)
∆E = 1/ρ(E) is the mean energy level spacing, ρ(E) is the mean level density
The quantum evolution follows the classical evolution including the chaotic diﬀusion
up to the Heisenberg time, at longer times the destructive interference sets in and
causes
the quantum or dynamical localization
Note: ρ(E) ∝ 1
(2π¯h)N → ∞ when ¯h → 0, and therefore eventually tH tT .
This observation applies to time-dependent and to time-independent systems.

We show the second moment p2
averaged over an ensemble of 106
initial
conditions uniformly distributed in the chaotic component on the interval
s ∈ [0, L/2] and p = 0.. We see that the saturation value of p2
is reached at about
NT = 105
collisions for λ = 0.15, NT = 103
collisions for λ = 0.20 and NT = 102
for
λ = 0.25. For λ = 0.15, according to the criterion at k = 2000 and k = 4000, we are
still in the regime where the dynamical localization is expected. On the other hand,
for λ = 0.20, 0.25 we expect extended states already at k < 2000.

2. Principle of Uniform Semiclassical Condensation (PUSC) of Wigner
functions of eigenstates (Percival 1973, Berry 1977, Shnirelman 1979, Voros 1979,
Robnik 1987-1998)
We study the structure of eigenstates in ”quantum phase space”: The Wigner
functions of eigenstates (they are real valued but not positive deﬁnite):
Deﬁnition: Wn(q, p) = 1
(2π¯h)N dN
X exp −i
¯hp.X ψn(q − X
2 )ψ∗
n(q + X
2 )
(P1) Wn(q, p)dN
p = |ψn(q)|2
(P2) Wn(q, p)dN
q = |φn(p)|2
(P3) Wn(q, p)dN
q dN
p = 1
(P4) (2π¯h)N
dN
q dN
pWn(q, p)Wm(q, p) = δnm
(P5) |Wn(q, p)| ≤ 1
(π¯h)N (Baker 1958)
(P6 = P4) W2
n(q, p)dN
q dN
p = 1
(2π¯h)N
(P7) ¯h → 0 : Wn(q, p) → (2π¯h)N
W2
n(q, p) > 0

In the semiclassical limit the Wigner functions condense on an element of phase
space of volume size (2π¯h)N
(elementary quantum Planck cell) and become positive
deﬁnite there.
Principle of Uniform Semiclassical Condensation (PUSC)
Wigner fun. Wn(q, p) condenses uniformly on a classically invariant component:
(C1) invariant N-torus (integrable or KAM): Wn(q, p) = 1
(2π)N δ (I(q, p) − In)
(C2) uniform on topologically transitive chaotic region:
Wn(q, p) = δ(En−H(q,p)) χω(q,p)
dNq dNp δ(En−H(q,p)) χω(q,p)
where χω(q, p) is the characteristic function on the chaotic component indexed by ω
(C3) ergodicity: microcanonical: Wn(q, p) = δ(En−H(q,p))
dNq dNp δ(En−H(q,p)
Important: Relative Liouville measure of the classical invariant component:
µ(ω) =
dN
q dN
p δ(En−H(q,p)) χω(q,p)
dNq dNp δ(En−H(q,p))

How good is this theory at suﬃciently small eﬀective ¯h?

4. Approach to describe the semiclassical transition regime
If we are not sufficiently deep in the semiclassical regime of sufficiently small effective
Planck constant ¯heff, which e.g. in billiards means not at sufficiently high energies,
we observe two new effects, which are the cause for the deviation from BR
statistics:
• Localization of eigenstates, due to the dynamical localization: The Wigner
functions are no longer uniformly spread over the classically available chaotic
component but are localized instead.
• Coupling due to tunneling between the semiclassical regular (R) and chaotic (C)
states
This effect typically disappears very quickly with increasing energy, due to the
exponential dependence on 1/¯heff.

Rough criterion for dynamical localization:
Heisenberg time tH = 2π¯h/(mean energy level spacing) = 2π¯h× (level density)
If the Heisenberg time tH is shorter than the classical diffusion time we observe the
localization, and extended (delocalized) states otherwise.
The Heisenberg time tH ∝ ¯h(1−N)
goes to infinity with ¯h → 0, therefore
asymptotically we always reach extended chaotic states and BR statistics.
But below the BR regime the effects of localization are observed, and can survive to
very high lying eigenstates, even up to one million above the ground state.
We shall illustrate the results in real billiard spectra.

Dynamically localized chaotic states are semiempirically well described by the
Brody level spacing distribution: (Izrailev 1988,1989, Prosen and Robnik1993/4)
PB(S) = C1Sβ
exp −C2Sβ+1
, FB(S) = 1 − WB(S) = exp −C2Sβ+1
,
where β ∈ [0, 1] and the two parameters C1 and C2 are determined by the two
normalizations < 1 >=< S >= 1, and are given by
C1 = (β + 1)C2, C2 = Γ β+2
β+1
β+1
with Γ(x) being the Gamma function. If we
have extended chaotic states β = 1 and RMT applies, whilst in the strongly localized
regime β = 0 and we have Poissonian statistics. The corresponding gap probability is
EB(S) =
1
(β + 1)Γ β+2
β+1
Q
1
β + 1
, Γ
β + 2
β + 1
S
β+1
Q(α, x) is the incomplete Gamma function: Q(α, x) =
∞
x
tα−1
e−t
dt.

The BRB theory: BR-Brody
(Prosen and Robnik 1993/1994, Batisti´c and Robnik 2010)
We have divided phase space µ1 + µ2 = 1 and localization β:
E(S) = Er(µ1S)Ec(µ2S) = exp(−µ1S)EBrody(µ2S)
and the level spacing distribution P(S) is:
P(S) =
d2
Er
dS2
Ec + 2
dEr
dS
dEc
dS
+ Er
d2
Ec
dS2

We study the billiard deﬁned by the quadratic complex conformal mapping:
w(z) = z + λz2
of the unit circle |z| = 1 (introduced in R. 1983/1984).
We chose λ = 0.15, for which ρ1 = 0.175
We plot the level spacing distribution P(S)

The level spacing distribution for the billiard λ = 0.15, compared with the analytical
formula for BRB (red full line) with parameter values ρ1 = 0.183, β = 0.465 and
σ = 0. The dashed red curve close to the full red line is BRB with classical
ρ1 = 0.175 is not visible, as it overlaps completely with the quantum case
ρ1 = 0.183. The dashed curve far away from the red full line is just the BR curve
with the classical ρ1 = 0.175. The Poisson and GOE curves (dotted) are shown for
comparison. The agreement of the numerical spectra with BRB is perfect. In the
histogram we have 650000 objects, and the statistical signiﬁcance is extremely large.

Discussion and conclusions
• The Principle of Uniform Semiclassical Condensation of Wigner functions of
eigenstates leads to the idea that in the suﬃciently deep semiclassical limit the
spectrum of a mixed type system can be described as a statistically independent
superposition of regular and chaotic level sequences.
• As a result of that the E(k, L) probabilities factorize and the level spacings and
other statistics can be calculated in a closed form.
• At lower energies we see quantum or dynamical localization.
• The level spacing distribution of localized chaotic eigenstates is excellently
described by the Brody distribution with β ∈ [0, 1].
• In the mixed type systems regular and chaotic eigenstates can be separated: the
regular obey Poisson, the localized chaotic states obey the Brody.
• The Brody level repulsion exponent β is a function of the localization measure A.

Acknowledgements
This work has been supported by the Slovenian Research Agency (ARRS).

6. References
Batistić B and Robnik M 2010 J. Phys. A: Math. Theor. 43 215101
Batistić B and Robnik M 2013 Phys. Rev. E 88 052913-1
Batistić B and Robnik M 2013 J. Phys. A: Math. Theor. 46 315102-1
Batistić B, Manos T and Robnik M 2013 Europhys. Lett. 102 50008-1
Berry M V 1985 Proc. Roy. Soc. Lond. A 400 229
Blümel R and Reinhardt W P 1997 Chaos in Atomic Physics (Cambridge University
Press)
Bohigas O, Giannoni M-J and Schmit C 1986 Lecture Notes in Physics 263 18
(Berlin: Springer)
Bohigas O, Giannoni M-J and Schmit C 1984 Phys. Rev. Lett. 52 1

Casati G and Chirikov B V 1995 Quantum Chaos (Cambridge University Press)
Casati G, Valz-Gris F and Guarneri I 1980 Lett. Nuovo Cimento 28 279
Faleiro E, Gomez J M G, Molina R A, Munoz L, Relano A and Retamosa J 2004
submitted to Phys. Rev. Lett. (arXiv:nlin.CD/0402028)
Friedrich H and Wintgen D 1989 Phys. Rep. 183 37-79
Gomez J M G, Relano A, Retamosa J, Faleiro E, Salasnich L, Vraniˇcar M and Robnik
M 2004 Phys. Rev. Lett. 94 084101
Grossmann S and Robnik M 2007 J. Phys A: Math. Theor. 40 409
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Manos T and Robnik M 2013 Phys. Rev. E 87 062905-1
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Robnik M 1982 J. Physique Colloque C2 43 45
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Robnik M 1998 Nonlinear Phenomena in Complex Systems (Minsk) 1 No 1, 1-22
Robnik M 2003a J.Phys.Soc.Jpn. 72 Suppl. C 81-86 (Proc. Waseda Int. Sympo. on
Fundamental Physics - New Perspectives in Quantum Physics)
Robnik M 2003b Preprint CAMTP/2 December 2003
Robnik M 2006 International Journal of Bifurcation and Chaos 16 No 6 1849
Robnik M and Romanovski V 2002 Nonlinear Phenomena in Complex Systems
(Minsk) 5 No4 445
Robnik M and Romanovski V 2003 J. Phys. A: Math. Gen. 36 7923
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(Berlin: Springer)
St¨ockmann H.-J. 1999 Quantum Chaos - An Introduction (Cambridge University

Press)
Vidmar G, St¨ockmann H.-J., Robnik M, Kuhl U, H¨ohmann R and Grossmann S 2007
J. Phys. A: Math. Theor. 40 13883

Quantum chaos of generic systems - Marko Robnik

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