spatially modulated phases in holography · • in condensed matter there is a variety of phases...
TRANSCRIPT
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Spatially Modulated Phases in Holography
Jerome GauntlettAristomenis Donos
Christiana Pantelidou
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Spatially Modulated Phases
• In condensed matter there is a variety of phases that are spatially modulated, spontaneously breaking translation invariance. For example: charge density waves and spin density waves
• The modulation is fixed by an order parameter associated with non-zero momentum .
• The modulation can be in various configurations such as stripes (as in the cuprates), in checkerboards and hexagonal lattices. Helical structure in chiral nematic liquid crystals and helimagnets e.g.
• There is a growing set of holographic examples described by exotic black holes (probe brane studies initiated by [Domokos,Harvey])
�O(k)� �= 0
MnSi
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• D=5 helical current phases [Nakamura,Ooguri,Park][Donos,Gauntlett]
• D=5 helical superconducting phases [Donos,Gauntlett]
• D=4 stripes [Donos,Gauntlett][Donos][Withers][Rozali,Smyth,Sorkin,Stang]
x3
x1
�Jx1� = 0
�Jx2� ∝ cos(kx1)
�Jx3� ∝ sin(kx1)
x2
�Jt� = const
�Jx� = 0�Jt� − Jt ∝ cos(2kx)�O� ∝ cos kx
�Jy� ∝ sin kx
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• Instabilities of unbroken phase black holes driven by mass squared becoming sufficiently negative
• For a single mode spatially modulation is suppressed
ω2 = mass2 + k2
k
Tc
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• However, instabilities for non-zero k can easily be achieved if there is a mixing of modes since one diagonalises a mass matrix
• The above examples achieve this via Chern Simons couplings and axions and one finds
Tc
kkc
• These examples all spontaneously break P and T
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• Not necessary: there are D=4,5 black holes dual CDWs that don’t break P and T [Donos,Gauntlett]
• The above examples are for CFTS at . There are also examples of spatially modulated phases in uniform magnetic fields [Bolognesi,Tong][Donos,Gauntlett,Pantelidou][Jokela,Lifschytz,Lippert][Cremonini,Sinkovics][Almuhairi,Polchinski][Ammon,Erdmenger,Shock,Strydom]....
• Closely related examples - but distinct physics - where translations broken explicitly [.....][Horowitz,Santos,Tong][Donos,Hartnoll][Vegh][Erdmenger,Ge,Pang][...]
• Many more examples of spatially modulated black holes to be found
• Finding them is one way of finding new ground states
T, µ
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• General results on the thermodynamics of periodic AdS black branes
• Competing superconducting p-wave and (p+ip)-wave orders
Plan
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Thermodynamics of Periodic AdS Black Branes
with Aristomenis Donos
Complementary work by [Domokos,Hoyos,Sonnenschien]
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• Consider asymptotic AdS black holes with planar topology.
• We are interested in solutions that are periodic in the spatial directions
Assume the black holes have a Killing horizon, dual to configurations in thermal equilibrium
Some of the configurations might be translationally invariant, independent of some or all of the spatial coordinates
If the translation symmetry is broken it can either be spontaneous orexplicit
• For simplicity consider bulk theory with metric and gauge-field g A
gmn ↔ Tµν Am ↔ Jµ
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Behaviour at the AdS boundary:
ds2 → γµνdxµdxν
• Bulk black brane solution is periodic in the globally defined with period . Might be compact or non-compact
xi
Li
• The black hole has a Killing horizon and the Killing vector on the boundary
xi
→ ∂t
The solutions might be independent of some
If solutions depend on the symmetry breaking can either be explicit if the sources or depend periodically on or spontaneous if not
xi
γµν xi
A → aµdxµ
xµ = (t, xi)• Introduce coordinates for d-dimensional boundary
aµ
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Euclideanise with and
We are interested in minimising free energy density
t → −iτ τ = τ +∆τ T−1 ≡ ∆τ
w = w (γµν , aµ;∆τ, Li) =1
∆τΠIOS (γµν , aµ;∆τ, Li)
Π ≡ ΠiLi
Variation with respect to and gives, as usual:γµν aµ
= − 1
Π
� {Li}
0dd−1x
√γ�12T
µν δγµν + Jµ δaµ�
Focus on the non-compact case.
δw = − 1
∆τΠ
� ∆τ
0
� {Li}
0dτdd−1x
√γ�12T
µν δγµν + Jµ δaµ�
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To get variation with respect to periods, scale coordinates:
τ = ∆τ τ xi = Li xi
with
IOS (γµν , aµ;∆τ, Li) = IOS (γµν , aµ; 1, 1)
and
ds2 → γµν dxµ dxν
≡ γττ (∆τ)2 dτ2 + 2γτxi∆τLidτdxi + γxixjLiLjdx
idxj
≡ aτ ∆τ dτ + axi Li dxi
A → aµdxµ
Variation with respect to periods via chain rule
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where
Comments:
1. For black branes invariant under translations in direction we have and this gives Smarr-type relation(s)Xi = 0
xi
c.f [El-Menoufi, Ett, Kastor,Traschen]
Xi = w +Π−1
� {L}
0dd−1x
√−γ (T txi
γtxi +�
j
T xixj
γxixj + Jxi
axi)
δw =−Π−1
� {L}
0dd−1x
√−γ
�12T
µν δγµν + Jµ δaµ�
− sδT −�
i
δLi
LiXi
s ≡ − 1
T
w +Π−1
� {L}
0dd−1x
√−γ(T ttγtt +
�
j
T txj
γtxj + J tat)
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2. Black branes that are spatially modulated in the direction, dependon wave-numbers . One has
xi
ki ≡ 2π/Li
kiδw
δki= Xi
The fact that this variation is simply related to and was obscure in a number of examples
Tµν Jµ
The thermodynamically preferred spatially modulated black branes in the non-compact case and where symmetry breaking is spontaneoushave Xi = 0
3. The expression for was a definition. It can be related to the area of the event horizon using bulk equations e.g. for two-derivative gravity it is1/4 of the area of the event horizon e.g [Papadimitriou,Skenderis]
S
= w +Π−1
� {L}
0dd−1x
√−γ(T txi
γtxi +�
j
T xixj
γxixj + Jxi
axi)
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Further relations can be obtained!
The euclidean boundary is a dimensional torus. The circle with tangent is singled out by the black hole in the bulk
d
Sl(d,Z)The transformation
τ = τ + αixi, no sum on i
xi = xi
with parametrises the same torus with same periods. αi =∆τ
Li
Also, ∂τ = ∂τ
∂τ
Can repeat the entire analysis in the barred coordinates - one should get the same result
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Remarkably, this implies
� {L}
0dd−1x
√−γ
�T xitγtt +
�
k
T xixk
γxkt + Jxi
at
�= 0
By considering other transformations preservingSl(d,Z) ∂τ
i �= j
� {L}
0dd−1x
�− det γ
�T xitγtxj +
�
k
T xixk
γxkxj + Jxi
axj
�= 0
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E.g. consider CFTs in flat spacetime, , γµν = ηµν aµ = (µ,0)
Assume spontaneous symmetry breaking in the direction.x1
Conservation of andTµν Jµ
T x1t, T x1x1
, . . . , T x1xd−1
, Jx1are constants
alsoδw = −J tδµ− sδT +
δk
k
�w + T x1x1
�
w = −T x2x2
= · · · = −T xd−1xd−1
w = −Ts− J tµ+ T tt
−T xit + Jxi
µ = 0
T xixj
= 0 i �= j �= 1
and
T x1xi
= 0
Bars refer to quantities averaged over a period
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• Results should generalise to other holographic scaling solutions such as Lifshitz
• Results can be generalised to include more matter fields
Some of these were not obvious from numerics!
Eg For thermodynamically preferred spatially modulated black branes
T x1x1
= −T x2x2
= · · · = −T xd−1xd−1
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Superconducting p-wave phases
withAristomenis Donos
Christiana Pantelidou
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Two approaches to study it holographically:
1. D=4,5 use SU(2) gauge fields.
Take the background to be charged with respect to and then spontaneously break the U(1) using the charged vector bosons [Gubser][Roberts,Hartnoll][Ammon,Erdmenger,Grass,Kerner,O’Bannon]
U(1) ⊂ SU(2)
In the specific setting it was shown that p-wave is preferred over (p+ip)-wave [Gubser, Pufu]
p-wave superconductivity is seen in a number of different systems e.g. , organic superconductors, He3 Sr2RuO4
2. D=5 use charged self-dual two-forms [Aprile,Franco,Rodriguez,Russo]
Extend p-wave studies of [Donos,Gauntlett] and develop (p+ip)-wave
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• The Charged two-form model in D=5
• The model admits a unit radius vacuum solution with which is dual to a d=4 CFT.
• The CFT has a global U(1) symmetry and is dual to the conserved current
• The two-form satisfies a self duality equation
and is dual to a d=4 self-dual tensor operator with charge and
L = (R+ 12) ∗ 1− 12 ∗ F ∧ F − 1
2 ∗ C ∧ C − i2mC ∧ H ,
∆(OC) = 2 +m
∗H = imC,
JµA
A = C = 0
F = dA, H = dC + ieA ∧ C .
e
AdS5
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• Such models arise in string theory. For example type IIB on can be truncated to this model with ,
• Electrically charged AdS-RN black brane describes the spatially homogeneous and isotropic phase of the CFT at , and high
e = 1/√3 m = 1
S5
UV: r → ∞ AdS4
IR: black hole horizon topology and temp
r → r+
At = µ(1− r+r)
Electric flux
R2
T
µ T
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• This model has superconducting instabilities if
• The simplest way to see this is to find modes that violating the BF bound of the T=0 limit of the AdS-RN black brane
• To determine the critical temperature at which the instability sets in, one looks for linearised normalisable zero modes in the full AdS-RN black brane solution
• Both p-wave and (p+ip)-wave instabilities depending on wave-number
• They spontaneously break the U(1) and some of the other translations and rotations....
AdS2
e2 >m2
2
k
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c3 = c03 +O (r − r+)
p-wave instabilities:
c3(r) ∼ cc3r−|m| + . . .
δC = · · ·+ c3(r) dx1 ∧ dx3
Order parameter points in the direction
Three translations preserved Rotations in the plane preserved
k = 0
(x1, x3)
x2
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Helical p-wave instabilities:
δC = · · ·+ c3(r) [sin(kx1)dx1 ∧ dx2 + cos(kx1)dx1 ∧ dx3]
x3
x1
k �= 0
preserved
This is the homogeneous Bianchi symmetry group
∂x2 ∂x3and
∂x1 + k(x3∂x2 − x2∂x3) preserved
V II0
x2
x2
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p+ip-wave instabilities
The phase of the order parameter is now involved
Three translations preserved Rotations in combined with gauge transformation preserved
δC = · · ·+ e−ikx1ic3(r)dx1 ∧ (dx2 − idx3)
δC = · · ·+ ic3(r)dx1 ∧ (dx2 − idx3)
p+ip-wave instabilities
Same symmetry as
(x2, x3)
k �= 0
k = 0
- translations in now combined with gauge transformations x1
k = 0
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m = 2P and (p+ip)-wave instabilities of AdS-RN for
�2 �1 0 1 2 3k
0.02
0.04
0.06
0.08
0.10
0.12T
e = 2
e = 2.8
e = 3.5
Highest T instability has k �= 0
Each point under bell curve corresponds to the existence of a back reacted p-wave and (p+ip)-wave black hole
For both cases we should find the preferred black holes which minimises the free energy density with respect to . Then we should compare p and (p+ip)
k
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• Ansatz
• Where are functions of and we have used the Bianchi invariant one-forms
• Solve ODEs for functions with suitable boundary conditions at the black hole horizon and at the AdS boundary. Analyse the thermodynamics....
ds2 = −g f2 dt2 + g−1dr2 + h2 ω21 + r2
�e2α ω2
2 + e−2α ω23
�
C = (i c1 dt+ c2dr) ∧ ω2 + c3 ω1 ∧ ω3
A = a dt
ω1 = dx1
ω2 = cos (kx1) dx2 − sin (kx1) dx3,
ω3 = cos (kx1) dx2 + sin (kx1) dx3
V II0
g, f, h,α, ci, a r
Back reacted Helical p-wave black holes
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0.0 0.5 1.0 1.5 2.0k
0.002
0.004
0.006
0.008
0.010
0.012
0.014
T
e = 2
0.02 0.04 0.06 0.08 0.10 0.12T0.0
0.2
0.4
0.6
0.8
1.0
cc3
Ttt = 3M + 8ch
Tx1x1 = M + 8ch
Tx2x2 = M + 8cα cos(2kx1)
Tx3x3 = M − 8cα cos(2kx1)
Tx2x3 = −8cα sin(2kx1)
Tx1x1 = Tx2x2 = Tx3x3
⇒ ch = 0
preferred branch:
∂kw = 0
⇒
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0.0 0.5 1.0 1.5 2.0k
0.002
0.004
0.006
0.008
0.010
0.012
0.014
T
e = 2
0.02 0.04 0.06 0.08 0.10 0.12T0.0
0.2
0.4
0.6
0.8
1.0
cc3
Ttt = 3M
Tx1x1 = M
Tx2x2 = M + 8cα cos(2kx1)
Tx3x3 = M − 8cα cos(2kx1)
Tx2x3 = −8cα sin(2kx1)
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• As we find that , with The solution interpolates between AdS5 in the UV and a helical scaling solution in the far IR:
Emergent helical scaling in the IR at T=0
T → 0
t → λzt, x2,3 → λx2,3, x1 → x1
r → λ−1r
ds2 = −(f20L
−2)r2zdt2 + L2 dr2
r2+ (k2h2
0)dx21 + r2
�e2α0 ω2
2 + e−2α0 ω23
�
C = . . .
A = . . .
s → T 2/z
where are constantsf0, L, h0,α0
Scaling
z ∼ 2
Similar to ground states of [Iuzuka,Kachru et al]
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�1 0 1 2 3k
0.01
0.02
0.03
0.04
0.05
0.06
0.07T
e = 2.8
Similar to the previous case, but now as we have
r → λ−1r, t → λzt, x1,3 → λ1−γx1,3, x2 → λ1+γx2
Similar to ground states of [Taylor]
T → 0 k → 0
ds2 = −(f20L
−2)r2zdt2 + L2 dr2
r2+ α−2
0 r2(1−γ)�dx2
1 + dx23
�+ α2
0r2(1+γ)dx2
2
New anisotropic scaling solution:
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�2 �1 0 1 2 3k
0.02
0.04
0.06
0.08
0.10
0.12T
e = 3.5 Similar to previous cases, but now we see the phenomenon of pitch inversion at Such pitch inversion is observed in chiral nematics and helimagnets.
Metric approaches AdS5 in the IR!
Similar behaviour was seen in s-wave superconductor [Horowitz, Roberts] and also in p-wave black holes for su(2) model [Basu]
Has been described as emergent conformal symmetry. However, correlators do not approach those of CFT for small frequency.
T �= 0
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ds2 = −gf2dt2 + g−1dr2 + h2(dx1 +Qdt)2 + r2(dx22 + dx2
3)
A = adt+ bdx1
C = e−ikx1(ic1dt+ c2dr + ic3dx1) ∧ (dx2 − idx3)
Time translations preserved, but stationary metric
Three space translations preserved (plus gauge)
Rotations in preserved (plus gauge)
Back reacted (p+ip)-wave black holes
(x2, x3)
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e = 2
0.02 0.04 0.06 0.08 0.10 0.12T0.0
0.2
0.4
0.6
0.8
1.0
cc3
Tx1x1 = Tx2x2 = Tx3x3
⇒ ch = 0
preferred branch:
∂kw = 0
⇒
Ttt = 3M + 8ch ,
Ttx1 = 4cQ ,
Tx1x1 = M + 8ch ,
Tx2x2 = M ,
Tx3x3 = M , Two extra Smarr relations
⇒ cQ = 0
0.0 0.5 1.0 1.5 2.0k
0.005
0.010
0.015T
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e = 2
0.02 0.04 0.06 0.08 0.10 0.12T0.0
0.2
0.4
0.6
0.8
1.0
cc3
Ttt = 3M
Ttx1 = 0
Tx1x1 = M
Tx2x2 = M
Tx3x3 = M
0.0 0.5 1.0 1.5 2.0k
0.005
0.010
0.015T
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e = 2.8
No analogue of pitch inversion
�1 0 1 2k
0.01
0.02
0.03
0.04
0.05
0.06
0.07T
�2 �1 0 1 2 3k
0.02
0.04
0.06
0.08
0.10
0.12T
e = 3.5
For all values of the charge we find as (in some cases at very low temperatures)
e s → 0 T → 0
The nature of the ground states is unclear....
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Competing orders
0.2 0.4 0.6 0.8 1.0T�Tc
�0.096
�0.094
�0.092
�0.090
�0.088
�0.086
�0.084
w
0.2 0.4 0.6 0.8 1.0T�Tc�0.30
�0.25
�0.20
�0.15
�0.10
we = 3.5
e = 2
p-wave preferred(p+ip)-wave preferred
0.0 0.2 0.4 0.6 0.8 1.0T�Tc�0.18
�0.17
�0.16
�0.15
�0.14
�0.13
�0.12
�0.11
w
e = 2.8(p+ip)-wave then first order transition to p-wave
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Final Comments
Rich classes of spatially modulated black holes exist with interesting properties and novel ground states
More to be discovered