Quantum criticality beyond the Landau-Ginzburg-Wilson …qpt.physics.harvard.edu/talks/sces.pdf ·...

Quantum criticality beyond the Landau-Ginzburg-Wilson paradigm

Leon Balents (UCSB)Lorenz Bartosch (Yale/Frankfurt)

Anton Burkov (UCSB)Matthew Fisher (UCSB)

Subir Sachdev (Yale)Krishnendu Sengupta (Yale)

T. Senthil (MIT)Ashvin Vishwanath (MIT)Matthias Vojta (Karlsruhe)

Phys. Rev. Lett. 90, 216403 (2003).Science 303, 1490 (2004).

cond-mat/0408xxxTalk online: Google Sachdev

( )( )

Collinear spins: 0Non-collinear spins: 0

× =× ≠

N NN N

T=0SDW

Pressure,carrier concentration,….

Quantum critical point

States on both sides of critical point could be either (A) Insulators

(B) Metals(C) Superconductors

SDWs in Mott insulators

2 4La CuO

( )4 / 3, 4 / 3K π π=Non-collinear spins

( ),K π π=Collinear spins

“Disorder” the spins by enhancing quantum fluctuations in a variety of ways…..

OutlineOutlineA. “Dimerized” Mott insulators

Landau-Ginzburg-Wilson (LGW) theory.

B. Kondo lattice models “Large” Fermi surfaces and the LGW SDW paramagnon theory.

C. Fractionalized Fermi liquidsSpin liquids and Fermi volume changing transitions with a topological order parameter.

D. Multiple order parameters LGW forbidden transitions

(A) Magnetic quantum phase transitions in “dimerized” Mott insulators

Landau-Ginzburg-Wilson (LGW) theory:Second-order phase transitions described by

fluctuations of an order parameterassociated with a broken symmetry

Coupled Dimer Antiferromagnet

ij SSJH ⋅= ∑><

10 ≤≤ λ

JλJM. P. Gelfand, R. R. P. Singh, and D. A. Huse, Phys. Rev. B 40, 10801-10809 (1989).N. Katoh and M. Imada, J. Phys. Soc. Jpn. 63, 4529 (1994).J. Tworzydlo, O. Y. Osman, C. N. A. van Duin, J. Zaanen, Phys. Rev. B 59, 115 (1999).M. Matsumoto, C. Yasuda, S. Todo, and H. Takayama, Phys. Rev. B 65, 014407 (2002).

close to 0λ Weakly coupled dimers

0, 0iS ϕ= =Paramagnetic ground state

( )↓↑−↑↓=2

Excitation: S=1 triplon

( )↓↑−↑↓=2

Excitation: S=1 triplon(exciton, spin collective mode)

Energy dispersion away fromantiferromagnetic wavevector

2 2 2 2

2x x y y

c p c pε

+= ∆ +

∆spin gap∆→

Coupled Dimer Antiferromagnet

ij SSJH ⋅= ∑><

10 ≤≤ λ

JλJM. P. Gelfand, R. R. P. Singh, and D. A. Huse, Phys. Rev. B 40, 10801-10809 (1989).N. Katoh and M. Imada, J. Phys. Soc. Jpn. 63, 4529 (1994).J. Tworzydlo, O. Y. Osman, C. N. A. van Duin, J. Zaanen, Phys. Rev. B 59, 115 (1999).M. Matsumoto, C. Yasuda, S. Todo, and H. Takayama, Phys. Rev. B 65, 014407 (2002).

close to 1λ Weakly dimerized square lattice

Excitations: 2 spin waves (magnons)

2 2 2 2p x x y yc p c pε = +

Ground state has long-range spin density wave (Néel) order at wavevector K= (π,π)

0 ϕ ≠

spin density wave order parameter: ; 1 on two sublatticesii i

ϕ η η= = ±

λc = 0.52337(3)M. Matsumoto, C. Yasuda, S. Todo, and H. Takayama,

Phys. Rev. B 65, 014407 (2002)T=0

λ 1 cλ Pressure in TlCuCl3

Quantum paramagnetNéel state

0ϕ ≠ 0ϕ =

The method of bond operators (S. Sachdev and R.N. Bhatt, Phys. Rev. B 41, 9323 (1990)) provides a quantitative description of spin excitations in TlCuCl3 across the quantum phase transition (M. Matsumoto, B. Normand, T.M. Rice, and M. Sigrist,

Phys. Rev. Lett. 89, 077203 (2002))

LGW theory for quantum criticalitywrite down an effective action

for the antiferromagnetic order parameter by expanding in powers of and its spatial and temporal d

Landau-Ginzburg-Wilson theor

erivatives, while preserving

ymmetries of the microscopic Hamiltonian

( ) ( ) ( )( ) ( )22 22 2 2 212 4!x c

ud xd cSϕ ττ ϕ ϕ λ λ ϕ ϕ⎡ ⎤= ∇ + ∂ + − +⎢ ⎥⎣ ⎦∫S. Chakravarty, B.I. Halperin, and D.R. Nelson, Phys. Rev. B 39, 2344 (1989)

( )2 2

c pp cε λ λ= ∆ + ∆ = −∆

( )For oscillations of about 0 lead to the following structure in the dynamic structure factor ,

S pλ λ ϕ ϕ

( ),S p ω

( )( )Z pδ ω ε−

Three triplon continuumTriplon pole

Structure holds to all orders in u

A.V. Chubukov, S. Sachdev, and J.Ye, Phys.

Rev. B 49, 11919 (1994)

(B) Kondo lattice models

“Large” Fermi surfaces and the Landau-Ginzburg-Wilson spin-density-wave

paramagnon theory

Kondo lattice

Local moments fσ Conduction electrons cσ† †

'K ij i j K i i fi fi fji j i ij

H t c c J c c S J S Sσ σ σ σσ στ<

= + ⋅ + ⋅∑ ∑ ∑

At large JK , magnetic order is destroyed, and we obtain a non-magnetic Fermi liquid (FL) ground state

S. Doniach, Physica B 91, 231 (1977).

Luttinger’s Fermi volume on a d-dimensional lattice for the FL phase

Let v0 be the volume of the unit cell of the ground state,nT be the total number density of electrons per volume v0.

(need not be an integer)

( )( )

02 Volume enclosed by Fermi surface2

1c cT fn n n n= + = +

A “large” Fermi surface

Argument for the Fermi surface volume of the FL phase

Single ion Kondo effect implies at low energiesKJ →∞

( )† † † † 0i i i ic f c f↑ ↓ ↓ ↑− † 0 , =1/2 holeif S↓

Fermi liquid of S=1/2 holes with hard-core repulsion

( )( ) ( )

Fermi surface volume density of holes mod 2

1 1 mod 2c cn n

= − − = +

Doniach’s T=0 phase diagram for the Kondo lattice

“Heavy” Fermi liquid with moments Kondo screened by conduction electrons.

Fermi surface volume equals the Luttinger value.

Local moments choose some static spin

arrangement

SDW FL

LGW theory for quantum critical point

( )( ) ( )( ) ( )2 22 2

K Kcdd qd uS q q J J d rdϕ

ω ϕ ω ω τ ϕπ += + + − +∫ ∫

Write down effective action for SDW order parameter ϕ

fluctuations are damped by mixing with fermionic quasiparticles near the Fermi surface

Fluctuations of about 0 the triplon is now a paramagno nϕ ϕ = ⇒J. Mathon, Proc. R. Soc. London A, 306, 355 (1968); T.V. Ramakrishnan, Phys. Rev. B 10, 4014 (1974); M. T. Beal-Monod and K. Maki, Phys. Rev. Lett. 34, 1461 (1975); J.A. Hertz, Phys. Rev. B 14, 1165 (1976).T. Moriya, Spin Fluctuations in Itinerant Electron Magnetism, Springer-Verlag, Berlin (1985); G. G. Lonzarich and L. Taillefer, J. Phys. C 18, 4339 (1985); A.J. Millis, Phys. Rev. B 48, 7183 (1993).

Doniach’s T=0 phase diagram for the Kondo lattice

Local moments choose some static spin arrangement.

Near the quantum critical point, the Fermi surface is modified

from the “large Fermi surface” only by the appearance of “gaps” near the hot spots.

SDW FL

(C) Fractionalized Fermi liquids (FL*)

Spin liquids and Fermi volume changing transitions with a topological order parameter

Beyond LGW: quantum phases and phase transitions with emergent gauge excitations

and fractionalization

Work in the regime with small JK, and consider destruction of magnetic order by frustrating

(RKKY) exchange interactions between f moments

Ground state has Neel order with 0ϕ ≠

Destroy SDW order by perturbations which preserve full square lattice symmetry e.g. second-neighbor or ring exchange.

A ground state with 0 and no broken lattice symmetries.

Such a state has emergent excitations described by a or U(1) gauge theory

spin liquid

P. Fazekas and P.W. Anderson, Phil Mag 30, 23 (1974). N. Read and S. Sachdev, Phys. Rev. Lett. 66, 1773 (1991); X. G. Wen, Phys. Rev. B 44, 2664 (1991).

Influence of conduction electrons

Local moments fσConduction electrons cσ

( ) ( )† †' ,ij i j K i i fi H fi fj

i j i i jH t c c J c c S J i j S Sσ σ σ σσ στ

= + ⋅ + ⋅∑ ∑ ∑

Determine the ground state of the quantum antiferromagnet defined by JH, and then couple to conduction electrons by JK

Choose JH so that ground state of antiferromagnet is a Z2 or U(1) spin liquid

Influence of conduction electrons

Conduction electrons cσLocal moments fσ

At JK= 0 the conduction electrons form a Fermi surface on their own with volume determined by nc.

Perturbation theory in JK is regular, and so this state will be stable for finite JK.So volume of Fermi surface is determined by

(nT -1)= nc(mod 2), and does not equal the Luttinger value.

The (U(1) or Z2) FL* state

A new phase: FL*

( )( )

02 Volume enclosed by Fermi surface2

1 mod 2

This phase preserves spin rotation invariance, and has a Fermi surface of sharp electron-like quasiparticles.

The state has “topological order” and associated neutral excitations. The topological order can be detected by the violation of Luttinger’s

Fermi surface volume. It can only appear in dimensions d > 1

Precursors: N. Andrei and P. Coleman, Phys. Rev. Lett. 62, 595 (1989).Yu. Kagan, K. A. Kikoin, and N. V. Prokof'ev, Physica B 182, 201 (1992).Q. Si, S. Rabello, K. Ingersent, and L. Smith, Nature 413, 804 (2001).S. Burdin, D. R. Grempel, and A. Georges, Phys. Rev. B 66, 045111 (2002).L. Balents and M. P. A. Fisher and C. Nayak, Phys. Rev. B 60, 1654, (1999); T. Senthil and M.P.A. Fisher, Phys. Rev. B 62, 7850 (2000).F. H. L. Essler and A. M. Tsvelik, Phys. Rev. B 65, 115117 (2002).

Phase diagram

U(1) FL* FL

JKc JK

Phase diagram

Fractionalized Fermi liquid with moments paired in a spin liquid. Fermi surface volume does not include

moments and is unequal to the Luttinger value.

U(1) FL* FL

JKc JK

Phase diagram

U(1) FL* FL

Phase diagram

U(1) FL* FL

Sharp transition at T=0 in compact U(1) gauge theory; compactness “irrelevant” at critical point

Phase diagram

FLU(1) FL*

Quantum Critical

No transition for T>0 in compact U(1) gauge theory; compactness essential for this feature

Sharp transition at T=0 in compact U(1) gauge theory; compactness “irrelevant” at critical point

Phase diagram

FLU(1) FL*

JKc JK

Quantum Critical

• Specific heat ~ T ln T• Violation of Wiedemann-FranzT

Phase diagram

FLU(1) FL*

JKc JK

Quantum Critical

( )Resistivity ~ 1/ ln 1/TT

Phase diagram (after allowing for conventional magnetic order)

Topological and SDW order parameters suggest two Topological and SDW order parameters suggest two separate quantum critical pointsseparate quantum critical points

(D) Multiple order parameters

Berry phases and the breakdown of the LGW paradigm

Ground state has Neel order with 0ϕ ≠

Possible paramagnetic ground state with 0ϕ =

Such a state breaks lattice symmetry and has 0, where is the

Ψ ≠

Ψ valence bond solid (VBS) order parameter

Ψ ≠

N. Read and S. Sachdev,

Phys. Rev. Lett. 62, 1694 (1989).

Ψ ≠

VBS order (and confinement) appear for collinear spins in d=2

Naïve approach: add VBS order parameter to LGW theory “by hand”

First order

transitionVBS

Neel order0, 0ϕ ≠ Ψ = VBS

VBS order0, 0ϕ = Ψ ≠

Coexistence0,

ϕ ≠

Ψ ≠VBS

( topologically ordered)

Disordered

= Ψ =VBS

Neel order0, 0ϕ ≠ Ψ =

First order

transitionVBS

Coexistence0,

ϕ ≠

Ψ ≠VBS

Disordered

= Ψ =VBS

Superfluid-insulator transition of hard core bosons at f=1/2 (Neel-valence bond solid transition of S=1/2 AFM)

A. W. Sandvik, S. Daul, R. R. P. Singh, and D. J. Scalapino, Phys. Rev. Lett. 89, 247201 (2002)Large scale (> 8000 sites) numerical study of the destruction of superfluid (i.e.

magnetic Neel) order at half filling with full square lattice symmetry

VBS insulator

Superfluid(Neel) order

( ) ( )i j i j i j k l i j k lij ijkl

H J S S S S K S S S S S S S S+ − − + + − + − − + − +

= + − +∑ ∑

Boson-vortex duality

Quantum mechanics of two-

dimensional bosons: world

lines of bosons in spacetime

Express theory of S=1/2 AFM as a theory of Sz= -1 “spin down” bosons at filling f=1/2

C. Dasgupta and B.I. Halperin, Phys. Rev. Lett. 47, 1556 (1981); D.R. Nelson, Phys. Rev. Lett. 60, 1973 (1988); M.P.A. Fisher and D.-H. Lee, Phys. Rev. B 39, 2756 (1989);

Classical statistical mechanics of a “dual” three-dimensional

superconductor:vortices in a

“magnetic” field

Express theory of S=1/2 AFM as a theory of Sz= -1 “spin down” bosons at filling f=1/2

Classical statistical mechanics of a “dual” three-dimensional

superconductor:vortices in a

“magnetic” field

Strength of “magnetic” field = density of bosons = f flux quanta per plaquette

Boson-vortex dualityStatistical mechanics of dual superconductor is invariant

under the square lattice space group:, : Translations by a lattice spacing in the , directions

: Rotation by 90 degrees.x yT T x y

1 1 1 4

Magnetic space group: ;

ifx y y x

y x x y

T T e T T

R T R T R T R T R

− − −

Strength of “magnetic” field = density of bosons = f flux quanta per plaquette

At density = / ( , relatively prime integers) there are species of vortices, (with =1 ), associated with gauge-equivalent regions of the Brillouin zone

f p q p qq

ϕ …

Hofstäder spectrum of dual “superconducting” order

1 1 1 4

Magnetic space group: ;

ifx y y x

y x x y

T T e T T

R T R T R T R T R

− − −

The vortices form a representation of the space group

i fx y

q projective

ϕ ϕ ϕ ϕ

→ →

→ ∑

Hofstäder spectrum of dual “superconducting” order

At density = / ( , relatively prime integers) there are species of vortices, (with =1 ), associated with gauge-equivalent regions of the Brillouin zone

f p q p qq

ϕ …

See also X.-G. Wen, Phys. Rev. B 65, 165113 (2002)

The fields characterize Neel (superfluid) and VBS orderbothϕ

Neel (superfluid) order: 0ϕ =

VBS (charge) order:

Status of space group symmetry determined by 2density operators at wavevectors ,

qi mnf i mf

ρ ϕ ϕ +=

= ∑i

( ) ( )

First order

transitionVBS

Coexistence0,

ϕ ≠

Ψ ≠VBS

Disordered

= Ψ =VBS

Predictions of extended “LGW” theory with projective symmetry

First order

transitionVBS

Coexistence0,

ϕ ≠

Ψ ≠VBS

Second order

transition

Phase diagram of S=1/2 square lattice antiferromagnet

Neel order~ 0z zα αβ βϕ σ ≠

VBSVBS order 0, 1/ 2 spinons confined, 1 triplon excitations

Ψ ≠=

Main lesson:

Novel second-order quantum critical point between phases with conventional order parameters.

A direct second-order transition between such phases is forbidden by symmetry in LGW theory.

Key question for metallic systems:

Is a direct second-order quantum critical point possible between metallic states distinguished by

two conventional order parameters: (A) SDW order(B) Shape of Fermi surface ?

Such a transition is obtained if the FL* phase is unstable to confinement to a SDW state at low

energies.

Phase diagram for the Kondo lattice ?

Local moments choose some static spin arrangement.

The shape of the Fermi surface differs strongly from that of the

heavy Fermi liquid

SDW FL

See also Q. Si, S. Rabello, K. Ingersent, and J. L. Smith, Nature 413, 804 (2001); S. Paschen, T. Luehmann, C. Langhammer, O. Trovarelli, S. Wirth, C. Geibel, F. Steglich,

Acta Physica Polonica B 34, 359 (2003).

Conclusions

Two possible routes to “exotic” quantum criticalityI. New FL* phase with a Fermi surface of electron-like

quasiparticles (whose volume violates the Luttinger theorem), topological order, emergent gauge excitations, and neutral fractionalized quasiparticles.

Novel Fermi-volume-changing quantum criticality in the transition between the FL and FL* phases (and associated SDW and SDW* phases).

Conclusions

Two possible routes to “exotic” quantum criticalityI. New FL* phase with a Fermi surface of electron-like

quasiparticles (whose volume violates the Luttinger theorem), topological order, emergent gauge excitations, and neutral fractionalized quasiparticles.

Novel Fermi-volume-changing quantum criticality in the transition between the FL and FL* phases (and associated SDW and SDW* phases).

Conclusions

Two possible routes to “exotic” quantum criticalityII. Conventional FL and SDW phases (but with very different

shapes of Fermi surfaces) undergo a direct quantum phase transition.

Analogous quantum critical point found in a direct transition between Neel and VBS states in S=1/2 Mott insulators in two dimensions. Mapping to this scenario to metals we obtain the above scenario if the FL* phase is unstable to confinement to a SDW phase.

Conclusions

Two possible routes to “exotic” quantum criticalityII. Conventional FL and SDW phases (but with very different

shapes of Fermi surfaces) undergo a direct quantum phase transition.

Analogous quantum critical point found in a direct transition between Neel and VBS states in S=1/2 Mott insulators in two dimensions. Mapping to this scenario to metals we obtain the above scenario if the FL* phase is unstable to confinement to a SDW phase.

Quantum criticality beyond the Landau-Ginzburg-Wilson …qpt.physics.harvard.edu/talks/sces.pdf ·...

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