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Breakdown of the Landau-Ginzburg-Wilson paradigm at quantum phase transitions
Science 303, 1490 (2004); cond-mat/0312617cond-mat/0401041
Leon Balents (UCSB) Matthew Fisher (UCSB)
T. Senthil (MIT) Ashvin Vishwanath (MIT)
Parent compound of the high temperature superconductors: 2 4La CuO
A Mott insulator
spin operator withangular momentum =1/2
ij i jij
i
H J S S
SS
=
⇒
∑ i
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
SS
ϕ η η= = ±
Parent compound of the high temperature superconductors: 2 4La CuO
A Mott insulator
spin operator withangular momentum =1/2
ij i jij
i
H J S S
SS
=
⇒
∑ i
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
SS
ϕ η η= = ±
Parent compound of the high temperature superconductors: 2 4La CuO
A Mott insulator
spin operator withangular momentum =1/2
ij i jij
i
H J S S
SS
=
⇒
∑ i
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
SS
ϕ η η= = ±
BCS
Doped state is a paramagnet with 0 and also a high temperature superconductor with the BCS pairing order parameter 0
With increasing , there must be one or more qua
.
nt
ϕ
δ
=
Ψ ≠
⇒
BCS
um phase transitions involving ( ) onset of a non-zero ( ) restoration of spin rotation invariance by a transition from 0 to 0
iii
ϕ ϕ
Ψ
≠ =
Introduce mobile carriers of density δby substitutional doping of out-of-plane
ions e.g. 2 4La Sr CuOδ δ−
Superconductivity in a doped Mott insulator
First study magnetic transition in Mott insulators………….
OutlineOutlineA. Magnetic quantum phase transitions in “dimerized”
Mott insulatorsLandau-Ginzburg-Wilson (LGW) theory
B. Mott insulators with spin S=1/2 per unit cellBerry phases, bond order, and the breakdown of the LGW paradigm
C. Technical detailsDuality and dangerously irrelevant operators
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
TlCuCl3
M. Matsumoto, B. Normand, T.M. Rice, and M. Sigrist, cond-mat/0309440.
Coupled Dimer AntiferromagnetM. 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).
S=1/2 spins on coupled dimers
JλJ
jiij
ij SSJH ⋅= ∑><
10 ≤≤ λ
close to 0λ Weakly coupled dimers
close to 0λ Weakly coupled dimers
0, 0iS ϕ= =Paramagnetic ground state
( )↓↑−↑↓=2
1
close to 0λ Weakly coupled dimers
( )↓↑−↑↓=2
1
Excitation: S=1 triplon
close to 0λ Weakly coupled dimers
( )↓↑−↑↓=2
1
Excitation: S=1 triplon
close to 0λ Weakly coupled dimers
( )↓↑−↑↓=2
1
Excitation: S=1 triplon
close to 0λ Weakly coupled dimers
( )↓↑−↑↓=2
1
Excitation: S=1 triplon
close to 0λ Weakly coupled dimers
( )↓↑−↑↓=2
1
Excitation: S=1 triplon
close to 0λ Weakly coupled dimers
( )↓↑−↑↓=2
1
Excitation: S=1 triplon(exciton, spin collective mode)
Energy dispersion away fromantiferromagnetic wavevector
2 2 2 2
2x x y y
p
c p c pε
+= ∆ +
∆spin gap∆ →
TlCuCl3
N. Cavadini, G. Heigold, W. Henggeler, A. Furrer, H.-U. Güdel, K. Krämer and H. Mutka, Phys. Rev. B 63 172414 (2001).
“triplon”
/
For quasi-one-dimensional systems, the triplon linewidth takesthe exact universal value 1.20 at low TBk T
Bk Te−∆=K. Damle and S. Sachdev, Phys. Rev. B 57, 8307 (1998)
This result is in good agreement with observations in CsNiCl3 (M. Kenzelmann, R. A. Cowley, W. J. L. Buyers, R. Coldea, M. Enderle, and D. F. McMorrow Phys. Rev. B 66, 174412 (2002)) and Y2NiBaO5 (G. Xu, C. Broholm, G. Aeppli, J. F. DiTusa, T.Ito, K. Oka, and H. Takagi, preprint).
Coupled Dimer Antiferromagnet
close to 1λ Weakly dimerized square lattice
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
SS
ϕ η η= = ±
TlCuCl3
J. Phys. Soc. Jpn 72, 1026 (2003)
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))
λc = 0.52337(3)M. Matsumoto, C. Yasuda, S. Todo, and H. Takayama,
Phys. Rev. B 65, 014407 (2002)T=0
λ 1 cλ δ in cuprates ?
Quantum paramagnet
0ϕ ≠ 0ϕ =
Néel state
Magnetic order as in La2CuO4 Electrons in charge-localized Cooper pairs
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
y:
all s
ϕϕ
ymmetries of the microscopic Hamiltonian
( ) ( ) ( ) ( )22 22 2 22
1 12 4!x c
ud xdc
Sϕ ττ ϕ ϕ λ λ ϕ ϕ⎡ ⎛ ⎞ ⎤= ∇ + ∂ + − +⎜ ⎟⎢ ⎥⎝ ⎠ ⎦⎣∫
S. Chakravarty, B.I. Halperin, and D.R. Nelson, Phys. Rev. B 39, 2344 (1989)
~3∆
( )2 2
; 2 c
c pp cε λ λ= ∆ + ∆ = −∆
( )For oscillations of about 0 lead to the following structure in the dynamic structure factor ,
c
S pλ λ ϕ ϕ
ω< =
ω
( ),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. Mott insulators with spin S=1/2 per unit cell:
Berry phases, bond order, and the breakdown of the LGW paradigm
Mott insulator with two S=1/2 spins per unit cell
Mott insulator with one S=1/2 spin per unit cell
Mott insulator with one S=1/2 spin per unit cell
Ground state has Neel order with 0ϕ ≠
Mott insulator with one S=1/2 spin per unit cell
Destroy Neel order by perturbations which preserve full square lattice symmetry e.g. second-neighbor or ring exchange.The strength of this perturbation is measured by a coupling g.
Small ground state has Neel order with 0
Large paramagnetic ground state with 0
g
g
ϕ
ϕ
⇒ ≠
⇒ =
Mott insulator with one S=1/2 spin per unit cell
Destroy Neel order by perturbations which preserve full square lattice symmetry e.g. second-neighbor or ring exchange.The strength of this perturbation is measured by a coupling g.
Small ground state has Neel order with 0
Large paramagnetic ground state with 0
g
g
ϕ
ϕ
⇒ ≠
⇒ =
Mott insulator with one S=1/2 spin per unit cell
Possible large paramagnetic gr Class ound state ( ) with 0A g ϕ =
Mott insulator with one S=1/2 spin per unit cell
bondΨ
Possible large paramagnetic gr Class ound state ( ) with 0A g ϕ =
( ) ( )arond
cb
tan j iii j
iji S S e −Ψ = ∑ i r r
bond bond
Such a state breaks the symmetry of rotations by / 2 about lattice sites,and has 0, where is the
nπΨ ≠ Ψ bond order parameter
Mott insulator with one S=1/2 spin per unit cell
( ) ( )arond
cb
tan j iii j
iji S S e −Ψ = ∑ i r r
bond bond
Such a state breaks the symmetry of rotations by / 2 about lattice sites,and has 0, where is the
nπΨ ≠ Ψ bond order parameter
bondΨ
ossible large paramagnetic gr Class ound state ( ) with 0A g ϕ =P
Mott insulator with one S=1/2 spin per unit cell
( ) ( )arond
cb
tan j iii j
iji S S e −Ψ = ∑ i r r
bond bond
Such a state breaks the symmetry of rotations by / 2 about lattice sites,and has 0, where is the
nπΨ ≠ Ψ bond order parameter
bondΨ
Possible large paramagnetic gr Class ound state ( ) with 0A g ϕ =
Mott insulator with one S=1/2 spin per unit cell
bondΨ
Possible large paramagnetic gr Class ound state ( ) with 0A g ϕ =
( ) ( )arond
cb
tan j iii j
iji S S e −Ψ = ∑ i r r
bond bond
Such a state breaks the symmetry of rotations by / 2 about lattice sites,and has 0, where is the
nπΨ ≠ Ψ bond order parameter
Mott insulator with one S=1/2 spin per unit cell
bondΨ
Possible large paramagnetic gr Class ound state ( ) with 0A g ϕ =
bond bond
Such a state breaks the symmetry of rotations by / 2 about lattice sites,and has 0, where is the
nπΨ ≠ Ψ bond order parameter
( ) ( )arond
cb
tan j iii j
iji S S e −Ψ = ∑ i r r
Mott insulator with one S=1/2 spin per unit cell
bond bond
Another state breaking the symmetry of rotations by / 2 about lattice sites,which also has 0, where is the
nπΨ ≠ Ψ bond order parameter
( ) ( )arond
cb
tan j iii j
iji S S e −Ψ = ∑ i r r
bondΨ
Possible large paramagnetic gr Class ound state ( ) with 0A g ϕ =
Mott insulator with one S=1/2 spin per unit cell
bond bond
Another state breaking the symmetry of rotations by / 2 about lattice sites,which also has 0, where is the
nπΨ ≠ Ψ bond order parameter
( ) ( )arond
cb
tan j iii j
iji S S e −Ψ = ∑ i r r
bondΨ
Possible large paramagnetic gr Class ound state ( ) with 0A g ϕ =
Mott insulator with one S=1/2 spin per unit cell
bond bond
Another state breaking the symmetry of rotations by / 2 about lattice sites,which also has 0, where is the
nπΨ ≠ Ψ bond order parameter
( ) ( )arond
cb
tan j iii j
iji S S e −Ψ = ∑ i r r
bondΨ
Possible large paramagnetic gr Class ound state ( ) with 0A g ϕ =
Mott insulator with one S=1/2 spin per unit cell
bond bond
Another state breaking the symmetry of rotations by / 2 about lattice sites,which also has 0, where is the
nπΨ ≠ Ψ bond order parameter
( ) ( )arond
cb
tan j iii j
iji S S e −Ψ = ∑ i r r
bondΨ
Possible large paramagnetic gr Class ound state ( ) with 0A g ϕ =
Mott insulator with one S=1/2 spin per unit cell
bond bond
Another state breaking the symmetry of rotations by / 2 about lattice sites,which also has 0, where is the
nπΨ ≠ Ψ bond order parameter
( ) ( )arond
cb
tan j iii j
iji S S e −Ψ = ∑ i r r
bondΨ
Possible large paramagnetic gr Class ound state ( ) with 0A g ϕ =
Resonating valence bonds
bond
Different valence bond pairings resonate with each other, leading to Cl
a resoass B
nating valenparamagnet)
ce bond , ( with 0
liquidΨ =
P. Fazekas and P.W. Anderson, Phil Mag 30, 23 (1974); P.W. Anderson 1987
Such states are associated with non-collinear spin correlations, Z2 gauge theory, and topological order.N. Read and S. Sachdev, Phys. Rev. Lett. 66, 1773 (1991); X. G. Wen, Phys. Rev. B 44, 2664 (1991).
Resonance in benzene leads to a symmetric configuration of valence
bonds (F. Kekulé, L. Pauling)
Excitations of the paramagnet with non-zero spin
bond 0; Class AΨ ≠
Excitations of the paramagnet with non-zero spin
bond 0; Class AΨ ≠
Excitations of the paramagnet with non-zero spin
bond 0; Class AΨ ≠
Excitations of the paramagnet with non-zero spin
bond 0; Class AΨ ≠
Excitations of the paramagnet with non-zero spin
bond 0; Class AΨ ≠
Excitations of the paramagnet with non-zero spin
bond 0; Class AΨ ≠
S=1/2 spinons, , are confined into a S=1
triplon, ϕ*~ z zα αβ βϕ σ
zα
Excitations of the paramagnet with non-zero spin
bond 0; Class AΨ ≠ bond 0; Class BΨ =
S=1/2 spinons, , are confined into a S=1
triplon, ϕ*~ z zα αβ βϕ σ
zα
Excitations of the paramagnet with non-zero spin
bond 0; Class AΨ ≠ bond 0; Class BΨ =
S=1/2 spinons, , are confined into a S=1
triplon, ϕ*~ z zα αβ βϕ σ
zα
Excitations of the paramagnet with non-zero spin
bond 0; Class AΨ ≠ bond 0; Class BΨ =
S=1/2 spinons, , are confined into a S=1
triplon, ϕ*~ z zα αβ βϕ σ
zα
Excitations of the paramagnet with non-zero spin
bond 0; Class AΨ ≠ bond 0; Class BΨ =
S=1/2 spinons, , are confined into a S=1
triplon, ϕ*~ z zα αβ βϕ σ
zα S=1/2 spinons can propagate
independently across the lattice
Quantum theory for destruction of Neel order
Ingredient missing from LGW theory: Ingredient missing from LGW theory: Spin Berry PhasesSpin Berry Phases
AiSAe
Quantum theory for destruction of Neel order
Ingredient missing from LGW theory: Ingredient missing from LGW theory: Spin Berry PhasesSpin Berry Phases
AiSAe
Quantum theory for destruction of Neel order
Quantum theory for destruction of Neel orderDiscretize imaginary time: path integral is over fields on the
sites of a cubic lattice of points a
Quantum theory for destruction of Neel orderDiscretize imaginary time: path integral is over fields on the
sites of a cubic lattice of points aa a
a
Recall = (0,0,1) in classical Neel state; 1 on two
square subl
2attices ;
a aSϕ η ϕη
→→ ±=
a+µϕ
0ϕ
aϕ
( ), ,x yµ τ=
Quantum theory for destruction of Neel orderDiscretize imaginary time: path integral is over fields on the
sites of a cubic lattice of points aa a
a
Recall = (0,0,1) in classical Neel state; 1 on two
square subl
2attices ;
a aSϕ η ϕη
→→ ±=
a+µϕ
0ϕ
aϕ
a a+ 0
oriented area of spherical triangle
formed by and an arbitrary reference , poi, nta hA alfµ
µϕ ϕ ϕ
→
2 aA µ
Quantum theory for destruction of Neel orderDiscretize imaginary time: path integral is over fields on the
sites of a cubic lattice of points aa a
a
Recall = (0,0,1) in classical Neel state; 1 on two
square subl
2attices ;
a aSϕ η ϕη
→→ ±=
a+µϕ
0ϕ
aϕ
a a+ 0
oriented area of spherical triangle
formed by and an arbitrary reference , poi, nta hA alfµ
µϕ ϕ ϕ
→
Quantum theory for destruction of Neel orderDiscretize imaginary time: path integral is over fields on the
sites of a cubic lattice of points aa a
a
Recall = (0,0,1) in classical Neel state; 1 on two
square subl
2attices ;
a aSϕ η ϕη
→→ ±=
a+µϕ
0ϕ
aϕ
a a+ 0
oriented area of spherical triangle
formed by and an arbitrary reference , poi, nta hA alfµ
µϕ ϕ ϕ
→
aγ
a µγ +
Quantum theory for destruction of Neel orderDiscretize imaginary time: path integral is over fields on the
sites of a cubic lattice of points aa a
a
Recall = (0,0,1) in classical Neel state; 1 on two
square subl
2attices ;
a aSϕ η ϕη
→→ ±=
a+µϕ
0ϕ
aϕ
a a+ 0
oriented area of spherical triangle
formed by and an arbitrary reference , poi, nta hA alfµ
µϕ ϕ ϕ
→
aγ
a µγ +
Quantum theory for destruction of Neel orderDiscretize imaginary time: path integral is over fields on the
sites of a cubic lattice of points aa a
a
Recall = (0,0,1) in classical Neel state; 1 on two
square subl
2attices ;
a aSϕ η ϕη
→→ ±=
a+µϕ
0ϕ
aϕ
a a+ 0
oriented area of spherical triangle
formed by and an arbitrary reference , poi, nta hA alfµ
µϕ ϕ ϕ
→
aγ
Change in choice of is like a “gauge transformation”
2 2a a a aA Aµ µ µγ γ+→ − +
0ϕ
a µγ +
Quantum theory for destruction of Neel orderDiscretize imaginary time: path integral is over fields on the
sites of a cubic lattice of points aa a
a
Recall = (0,0,1) in classical Neel state; 1 on two
square subl
2attices ;
a aSϕ η ϕη
→→ ±=
a+µϕ
0ϕ
aϕ
a a+ 0
oriented area of spherical triangle
formed by and an arbitrary reference , poi, nta hA alfµ
µϕ ϕ ϕ
→
aγ
Change in choice of is like a “gauge transformation”
2 2a a a aA Aµ µ µγ γ+→ − +
0ϕ
The area of the triangle is uncertain modulo 4π, and the action has to be invariant under 2a aA Aµ µ π→ +
S. Sachdev and K. Park, Annals of Physics, 298, 58 (2002)
Quantum theory for destruction of Neel order
Ingredient missing from LGW theory: Ingredient missing from LGW theory: Spin Berry PhasesSpin Berry Phases
exp a aa
i A τη⎛ ⎞⎜ ⎟⎝ ⎠
∑Sum of Berry phases of all spins on the square lattice.
, exp
with "current" of
charges 1 on sublattices
a aa
a
i J A
J
static
µ µµ
µ
⎛ ⎞= ⎜ ⎟
⎝ ⎠
±
∑
Quantum theory for destruction of Neel order
( )2
,
11 expa a a a a aa aa
Z d i Ag µ τ
µ
ϕ δ ϕ ϕ ϕ η+
⎛ ⎞= − ⋅ +⎜ ⎟
⎝ ⎠∑ ∑∏∫
Partition function on cubic lattice
Modulus of weights in partition function: those of a classical ferromagnet at a “temperature” g
Small ground state has Neel order with 0
Large paramagnetic ground state with 0 Berry phases lead to large cancellations between different time histories need an effective action for a
g
g
A
ϕ
ϕ
⇒ ≠
⇒ =
→ at large gµ
Simplest large g effective action for the Aaµ
( )2
2 2
,
withThis is compact QED in 3 spacetime dimensions with
static charges 1 on
1exp c
two sublat
tices.
o2
~
sa a a a aaa
Z dA A A i Ae
e g
µ µ ν ν µ τµ
η⎛ ⎞= ∆ − ∆ +⎜ ⎟⎝ ⎠
±
∑ ∑∏∫
N. Read and S. Sachdev, Phys. Rev. Lett. 62, 1694 (1989).S. Sachdev and R. Jalabert, Mod. Phys. Lett. B 4, 1043 (1990).
S. Sachdev and K. Park, Annals of Physics, 298, 58 (2002)
N. Read and S. Sachdev, Phys. Rev. Lett. 62, 1694 (1989).
For large e2 , low energy height configurations are in exact one-to-one correspondence with nearest-neighbor valence bond pairings of the sites square lattice
There is no roughening transition for three dimensional interfaces, which are smooth for all couplings
There is a definite average height of the interfaceGround state has bond order.
⇒⇒
N. Read and S. Sachdev, Phys. Rev. Lett. 62, 1694 (1989).
( )2
,
11 expa a a a a aa aa
Z d i Ag µ τ
µ
ϕ δ ϕ ϕ ϕ η+
⎛ ⎞= − ⋅ +⎜ ⎟
⎝ ⎠∑ ∑∏∫
g0
Neel order 0ϕ ≠
?bond
Bond order0
Not present in LGW theory of orderϕ
Ψ ≠
or
Naïve approach: add bond order parameter to LGW theory “by hand”
First order
transitionbond
Neel order0, 0ϕ ≠ Ψ = bond
Bond order0, 0ϕ = Ψ ≠
g
gbond
Coexistence0,
0
ϕ ≠
Ψ ≠bond
Neel order0, 0ϕ ≠ Ψ = bond
Bond order0, 0ϕ = Ψ ≠
gbond
"disordered"0,
0
ϕ =
Ψ =bond
Neel order0, 0ϕ ≠ Ψ =
bond
Bond order0, 0ϕ = Ψ ≠
Bond order in a frustrated S=1/2 XY magnet
A. W. Sandvik, S. Daul, R. R. P. Singh, and D. J. Scalapino, Phys. Rev. Lett. 89, 247201 (2002)
First large scale (> 8000 spins) numerical study of the destruction of Neel order in a S=1/2 antiferromagnet with full square lattice symmetry
( ) ( )2 x x y yi j i j i j k l i j k l
ij ijklH J S S S S K S S S S S S S S+ − + − − + − +
⊂
= + − +∑ ∑g=
( )2
,
11 expa a a a a aa aa
Z d i Ag µ τ
µ
ϕ δ ϕ ϕ ϕ η+
⎛ ⎞= − ⋅ +⎜ ⎟
⎝ ⎠∑ ∑∏∫
g0
Neel order 0ϕ ≠
?bond
Bond order0
Not present in LGW theory of orderϕ
Ψ ≠
or
g0S. Sachdev and R. Jalabert, Mod. Phys. Lett. B 4, 1043 (1990). S. Sachdev and K. Park, Annals of Physics 298, 58 (2002).
? or
S. Sachdev and R. Jalabert, Mod. Phys. Lett. B 4, 1043 (1990); G. Murthy and S. Sachdev, Nuclear Physics B 344, 557 (1990); C. Lannert, M.P.A. Fisher, and T. Senthil, Phys. Rev. B 63, 134510 (2001); S. Sachdev and K. Park, Annals of Physics, 298, 58 (2002); O. Motrunich and A. Vishwanath, cond-mat/0311222.
Theory of a second-order quantum phase transition between Neel and bond-ordered phases
*
At the quantum critical point: +2 periodicity can be ignored
(Monopoles interfere destructively and are dangerously irrelevant). =1/2 , with ~ , are globally
pro
A A
S spinons z z z
µ µ
α α αβ β
π
ϕ σ
• →
•
pagating degrees of freedom.
Second-order critical point described by emergent fractionalized degrees of freedom (Aµ and zα );
Order parameters (ϕ and Ψbond ) are “composites” and of secondary importance
Second-order critical point described by emergent fractionalized degrees of freedom (Aµ and zα );
Order parameters (ϕ and Ψbond ) are “composites” and of secondary importance
→
T. Senthil, A. Vishwanath, L. Balents, S. Sachdev and M.P.A. Fisher, Science 303, 1490 (2004).
Phase diagram of S=1/2 square lattice antiferromagnet
g*
Neel order
~ 0z zα αβ βϕ σ ≠
(associated with condensation of monopoles in ),Aµ
or
bondBond order 0Ψ ≠
1/ 2 spinons confined, 1 triplon excitations
S zS
α==
T. Senthil, A. Vishwanath, L. Balents, S. Sachdev and M.P.A. Fisher, Science 303, 1490 (2004). S. Sachdev cond-mat/0401041.
(Quadrupled) monopole fugacity
Bond order
B. Mott insulators with spin S=1/2 per unit cell:
Berry phases, bond order, and the breakdown of the LGW paradigmOrder parameters/broken symmetry
+Emergent gauge excitations, fractionalization.
C. Technical details
Duality and dangerously irrelevant operators
Nature of quantum critical point
Use a sequence of simpler models which can be analyzed byduality mappings
A. Non-compact QED with scalar matterB. Compact QED with scalar matterC. N=1: Compact QED with scalar matter and Berry phasesD. theoryE. Easy plane case for N=2
N → ∞
Nature of quantum critical point
Use a sequence of simpler models which can be analyzed byduality mappings
A. Non-compact QED with scalar matterB. Compact QED with scalar matterC. N=1: Compact QED with scalar matter and Berry phasesD. theoryE. Easy plane case for N=2
N → ∞
A. N=1, non-compact U(1), no Berry phases
C. Dasgupta and B.I. Halperin, Phys. Rev. Lett. 47, 1556 (1981).
Nature of quantum critical point
Use a sequence of simpler models which can be analyzed byduality mappings
A. Non-compact QED with scalar matterB. Compact QED with scalar matterC. N=1: Compact QED with scalar matter and Berry phasesD. theoryE. Easy plane case for N=2
N → ∞
Nature of quantum critical point
Use a sequence of simpler models which can be analyzed byduality mappings
A. Non-compact QED with scalar matterB. Compact QED with scalar matterC. N=1: Compact QED with scalar matter and Berry phasesD. theoryE. Easy plane case for N=2
N → ∞
B. N=1, compact U(1), no Berry phases
Nature of quantum critical point
Use a sequence of simpler models which can be analyzed byduality mappings
A. Non-compact QED with scalar matterB. Compact QED with scalar matterC. N=1: Compact QED with scalar matter and Berry phasesD. theoryE. Easy plane case for N=2
N → ∞
Nature of quantum critical point
Use a sequence of simpler models which can be analyzed byduality mappings
A. Non-compact QED with scalar matterB. Compact QED with scalar matterC. N=1: Compact QED with scalar matter and Berry phasesD. theoryE. Easy plane case for N=2
N → ∞
C. N=1, compact U(1), Berry phases
C. N=1, compact U(1), Berry phases
C. N=1, compact U(1), Berry phases
Nature of quantum critical point
Use a sequence of simpler models which can be analyzed byduality mappings
A. Non-compact QED with scalar matterB. Compact QED with scalar matterC. N=1: Compact QED with scalar matter and Berry phasesD. theoryE. Easy plane case for N=2
N → ∞
Identical critical theories !
Nature of quantum critical point
Use a sequence of simpler models which can be analyzed byduality mappings
A. Non-compact QED with scalar matterB. Compact QED with scalar matterC. N=1: Compact QED with scalar matter and Berry phasesD. theoryE. Easy plane case for N=2
N → ∞
Identical critical theories !
D. , compact U(1), Berry phasesN → ∞
E. Easy plane case for N=2
Phase diagram of S=1/2 square lattice antiferromagnet
g*
Neel order
~ 0z zα αβ βϕ σ ≠
(associated with condensation of monopoles in ),Aµ
or
bondBond order 0Ψ ≠
1/ 2 spinons confined, 1 triplon excitations
S zS
α==
T. Senthil, A. Vishwanath, L. Balents, S. Sachdev and M.P.A. Fisher, Science 303, 1490 (2004). S. Sachdev cond-mat/0401041.
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