Quantum phase transitions in condensed matter

Transcription

1 Quantum phase transitions in condensed matter The 8th Asian Winter School on Strings, Particles, and Cosmology, Puri, India January 11-18, 2014 Subir Sachdev Talk online: sachdev.physics.harvard.edu HARVARD

2 Outline 1. The simplest models without quasiparticles A. Superfluid-insulator transition of ultracold bosons in an optical lattice B. Conformal field theories in 2+1 dimensions and the AdS/CFT correspondence 2. Metals without quasiparticles A. Review of Fermi liquid theory B. A non-fermi liquid: the Ising-nematic quantum critical point C. The holographic view: charged black-branes

3 Outline 1. The simplest models without quasiparticles A. Superfluid-insulator transition of ultracold bosons in an optical lattice B. Conformal field theories in 2+1 dimensions and the AdS/CFT correspondence 2. Metals without quasiparticles A. Review of Fermi liquid theory B. A non-fermi liquid: the Ising-nematic quantum critical point C. The holographic view: charged black-branes

4 Begin with a CFT

5 Holographic representation: AdS4 A 2+1 dimensional CFT at T=0 S = Z d 4 x p g apple 1 2apple 2 R + 6L 2

6 Holographic representation: AdS4 A 2+1 dimensional CFT at T=0 2 apple L dr ds 2 2 = r f(r) with f(r) =1 f(r)dt 2 + dx 2 + dy 2

7 Apply a chemical potential

8 AdS4 theory of nearly perfect fluids To leading order in a gradient expansion, charge transport in an infinite set of strongly-interacting CFT3s can be described by Einstein-Maxwell gravity/electrodynamics on AdS 4 -Schwarzschild Z S EM = d 4 x p apple 1 g F ab F ab. 4g 2 4 This is to be solved subject to the constraint A µ (r! 0,x,y,t)=A µ (x, y, t) where A µ is a source coupling to a conserved U(1) current J µ of the CFT3 Z S = S CFT + i dxdydta µ J µ At non-zero chemical potential we simply require A = µ.

9 AdS4 theory of nearly perfect fluids To leading order in a gradient expansion, charge transport in an infinite set of strongly-interacting CFT3s can be described by Einstein-Maxwell gravity/electrodynamics on AdS 4 -Schwarzschild Z S EM = d 4 x p apple 1 g F ab F ab. 4g 2 4 This is to be solved subject to the constraint A µ (r! 0,x,y,t)=A µ (x, y, t) where A µ is a source coupling to a conserved U(1) current J µ of the CFT3 Z S = S CFT + i dxdydta µ J µ At non-zero chemical potential we simply require A = µ.

10 The Maxwell-Einstein theory of the applied chemical potential yields a AdS4-Reissner-Nordtröm black-brane r E r = hqi Electric flux hqi =0 S = Z d 4 x p g apple 1 2apple 2 E r = hqi R + 6L 2 1 4g 2 4 F ab F ab S. A. Hartnoll, P. K. Kovtun, M. Müller, and S. Sachdev, Physical Review B 76, (2007)

11 The Maxwell-Einstein theory of the applied chemical potential yields a AdS4-Reissner-Nordtröm black-brane r E r = hqi Electric flux E r = hqi hqi =0 ds 2 = L r with f(r) = 2 apple dr 2 1 f(r) r R f(r)dt 2 + dx 2 + dy r R + 3r2 R 2 and R = p 6Lg4 appleµ, and A = µ 1 r R

12 The Maxwell-Einstein theory of the applied chemical potential yields a AdS4-Reissner-Nordtröm black-brane r Electric flux hqi =0 At T = 0, we obtain an extremal black-brane, with a near-horizon (IR) metric of AdS 2 R 2 ds 2 = L2 6 dt 2 + dr 2 r 2 + dx 2 + dy 2 T. Faulkner, H. Liu, J. McGreevy, and D. Vegh, arxiv:

13 Holography of a non-fermi liquid Einstein-Maxwell-dilaton theory r E r = hqi Electric flux S = Z d d+2 x p g apple 1 2apple 2 E r = hqi R 2(r ) 2 V ( ) Z( ) L 2 4e 2 F abf ab with Z( ) = Z 0 e, V ( ) = V 0 e, as!1. C. Charmousis, B. Gouteraux, B. S. Kim, E. Kiritsis and R. Meyer, JHEP 1011, 151 (2010). S. S. Gubser and F. D. Rocha, Phys. Rev. D 81, (2010). N. Iizuka, N. Kundu, P. Narayan and S. P. Trivedi, arxiv: [hep-th].

14 Holography of a non-fermi liquid ds 2 = 1 dt 2 r 2 r 2d(z 1)/(d ) + r2 /(d ) dr 2 + dx 2 i The r!1limit of the metric of the Einstein-Maxwelldilaton (EMD) theory has the above form with = d 2 +(d 1) z = 1+ d + 8(d(d )+ )2 d 2 (d ) 2.

15 Holography of a non-fermi liquid ds 2 = 1 dt 2 r 2 r 2d(z 1)/(d ) + r2 /(d ) dr 2 + dx 2 i This is the most general metric which is invariant under the scale transformation x i! x i t! z t ds! /d ds. This identifies z as the dynamic critical exponent (z = 1 for relativistic quantum critical points). We will see shortly that is the violation of hyperscaling exponent. We have used reparametrization invariance in r to define it so that it scales as r! (d )/d r. L. Huijse, S. Sachdev, B. Swingle, Physical Review B 85, (2012)

16 Holography of a non-fermi liquid ds 2 = 1 dt 2 r 2 r 2d(z 1)/(d ) + r2 /(d ) dr 2 + dx 2 i At T>0, there is a black-brane at r = r h. The Beckenstein-Hawking entropy of the black-brane is the thermal entropy of the quantum system r = 0. The entropy density, S, is proportional to the area of the horizon, and so S r d h r L. Huijse, S. Sachdev, B. Swingle, Physical Review B 85, (2012)

17 Holography of a non-fermi liquid ds 2 = 1 dt 2 r 2 r 2d(z 1)/(d ) + r2 /(d ) dr 2 + dx 2 i Under rescaling r! (d )/d r, and the temperature T t 1, and so S T (d )/z = T d eff /z where = d d e, the dimension deficit, is now identified as the violation of hyperscaling exponent. r L. Huijse, S. Sachdev, B. Swingle, Physical Review B 85, (2012)

18 Holography of a non-fermi liquid ds 2 = 1 dt 2 r 2 r 2d(z 1)/(d ) + r2 /(d ) dr 2 + dx 2 i The null energy condition (stability condition for gravity) yields a new inequality z 1+ d In d = 2, with = d 1, this implies z 3/2. Sothelower bound is precisely the value obtained from the field theory. N. Ogawa, T. Takayanagi, and T. Ugajin, JHEP 1201, 125 (2012). L. Huijse, S. Sachdev, B. Swingle, Physical Review B 85, (2012)

19 Holography of a non-fermi liquid ds 2 = 1 dt 2 r 2 r 2d(z 1)/(d ) + r2 /(d ) dr 2 + dx 2 i Application of the Ryu-Takayanagi minimal area formula to a dual Einstein-Maxwell-dilaton theory yields 8 < P, for <d 1 S E P ln P, for = d 1. : P /(d 1), for >d 1 The log-violation of area law again prefers the value = d 1. Moreover, the co-e cient of P ln P is (i) independent of the shape of the entangling region just as expected for a circular Fermi surface, and (ii) has the same universal dependence on Q expected from the Luttinger theorem. N. Ogawa, T. Takayanagi, and T. Ugajin, JHEP 1201, 125 (2012). L. Huijse, S. Sachdev, B. Swingle, Physical Review B 85, (2012)

20 Open questions: Holography of a non-fermi liquid Is there any selection principle for the values of and z? What is the physical interpretation of metallic states with 6= d 1? Does the metallic state have a Fermi surface, and what is k F? Are there N 2 Fermi surfaces of quarks with k F 1, or 1 Fermi surface of a baryon with k F N 2? Why is k F not observable as Friedel oscillations in correlators of the density, and other gauge-neutral operators? Answer: need non-perturbative e ects of monopole operators T. Faulkner and N. Iqbal, arxiv: ; S. Sachdev, Phys. Rev. D 86, (2012)

21 Open questions: Holography of a non-fermi liquid Is there any selection principle for the values of and z? What is the physical interpretation of metallic states with 6= d 1? Does the metallic state have a Fermi surface, and what is k F? Are there N 2 Fermi surfaces of quarks with k F 1, or 1 Fermi surface of a baryon with k F N 2? Why is k F not observable as Friedel oscillations in correlators of the density, and other gauge-neutral operators? Answer: need non-perturbative e ects of monopole operators T. Faulkner and N. Iqbal, arxiv: ; S. Sachdev, Phys. Rev. D 86, (2012)

22 Open questions: Holography of a non-fermi liquid Is there any selection principle for the values of and z? What is the physical interpretation of metallic states with 6= d 1? Does the metallic state have a Fermi surface, and what is k F? Are there N 2 Fermi surfaces of quarks with k F 1, or 1 Fermi surface of a baryon with k F N 2? Why is k F not observable as Friedel oscillations in correlators of the density, and other gauge-neutral operators? Answer: need non-perturbative e ects of monopole operators T. Faulkner and N. Iqbal, arxiv: ; S. Sachdev, Phys. Rev. D 86, (2012)

23 Open questions: Holography of a non-fermi liquid Is there any selection principle for the values of and z? What is the physical interpretation of metallic states with 6= d 1? Does the metallic state have a Fermi surface, and what is k F? Are there N 2 Fermi surfaces of quarks with k F 1, or 1 Fermi surface of a baryon with k F N 2? Why is k F not observable as Friedel oscillations in correlators of the density, and other gauge-neutral operators? Answer: need non-perturbative e ects of monopole operators T. Faulkner and N. Iqbal, arxiv: ; S. Sachdev, Phys. Rev. D 86, (2012)

24 Open questions: Holography of a non-fermi liquid Is there any selection principle for the values of and z? What is the physical interpretation of metallic states with 6= d 1? Does the metallic state have a Fermi surface, and what is k F? Are there N 2 Fermi surfaces of quarks with k F 1, or 1 Fermi surface of a baryon with k F N 2? Why is k F not observable as Friedel oscillations in correlators of the density, and other gauge-neutral operators? Answer: need non-perturbative e ects of monopole operators T. Faulkner and N. Iqbal, arxiv: ; S. Sachdev, Phys. Rev. D 86, (2012)

25 R. A. Davison, M. Goykhman, and A. Parnachev, arxiv: Consider the truncation of IIB supergravity on AdS 5 S 5 where two of the three U(1) charges are equal and non-vanishing while the third one is zero (S. S. Gubser and F. D. Rocha, Phys. Rev. D 81, (2010)). In the IR limit, the bulk metric is of the general scaling form, but with = z and z!1: ds 2 = 1 r 2 dt 2 r 6 + dr2 r 2 + dx2 i This metric is conformal to AdS 2 R 3. From our results before, we have the entropy S T and the entanglement entropy S E P. Key di erence from a Landau Fermi liquid are the equality of hydrodynamic and zero sound velocities, and a viscosity = S/(4 )..

26 R. A. Davison, M. Goykhman, and A. Parnachev, arxiv: Claim: all physical properties of the holographic theory can be interpreted in a theory of a Fermi surface of baryons with k F N 2/3, v F N 2/3, and interactions such that the system is precisely at the nematic quantum critical point in d = 3!

27 Strongly-coupled quantum criticality leads to a novel regime of quantum dynamics without quasiparticles. The simplest examples are conformal field theories in 2+1 dimensions, realized by ultracold atoms in optical lattices. Holographic theories provide an excellent quantitative description of quantum Monte studies of quantum-critical boson models Exciting recent progress on the description of transport in metallic states without quasiparticles, via field theory and holography

28 Strongly-coupled quantum criticality leads to a novel regime of quantum dynamics without quasiparticles. The simplest examples are conformal field theories in 2+1 dimensions, realized by ultracold atoms in optical lattices. Holographic theories provide an excellent quantitative description of quantum Monte studies of quantum-critical boson models Exciting recent progress on the description of transport in metallic states without quasiparticles, via field theory and holography

29 Strongly-coupled quantum criticality leads to a novel regime of quantum dynamics without quasiparticles. The simplest examples are conformal field theories in 2+1 dimensions, realized by ultracold atoms in optical lattices. Holographic theories provide an excellent quantitative description of quantum Monte studies of quantum-critical boson models Exciting recent progress on the description of transport in metallic states without quasiparticles, via field theory and holography

30 Strongly-coupled quantum criticality leads to a novel regime of quantum dynamics without quasiparticles. The simplest examples are conformal field theories in 2+1 dimensions, realized by ultracold atoms in optical lattices. Holographic theories provide an excellent quantitative description of quantum Monte studies of quantum-critical boson models Exciting recent progress on the description of transport in metallic states without quasiparticles, via field theory and holography