Sung-Sik Lee (McMaster U and Perimeter Institute, Canada)

From renormalization group to emergent gravity: holographic description of quantum many-body systems

Blogged by Piers Coleman.

Sung-Sik begins talking about examples of scs, CM systems, high Tc, heavy fermion systems near a QCP, but alos QCD, the quark gluon plasma.

The long distance, low energy physics is described by a strongly interacting QFT.  We need a new way of approaching these problems. 

One new approach he suggests, is "Duality", the idea that one theory can be mapped onto another. For example, the 3D xy model can be mapped to a U(1) gauge theory w charged boson. EM duality in 4D gauge theories.

The hope: find a new way of mapping strongly coupled theories onto weakly coupled theories, using duality.  This kind of thing can happen if 

Original particles remain strongly coupled and have a short life time, yet organized into long-lived, weakly coupled collective excitations

Non-trivial dynamical info contained in the change of variable

Dual variable may carry new, sometimes fractional quantum numbers

It may live in a different space. 

Q: when doesn't it work?
A: it doesn't work in MOST cases, but I will tell you about a case where it may! Holography.

Holography: AdS/CFT correspondence.   Here the bold new idea, due to Maldacena, is that a D-dimensional AFT is dual ot a D+1 dimensional gravity theory.

• N=4 SU(N) gauge theory in 4D = 11B superstring theory in AdS5xS5
• Weak coupling description for strongly coupled QFT for a large N 
• Believed to be a general framework for a large class of qFs
• The correspondence has been used to "reporoduce" many phenomena in CMT - from hydrodynamics to SC and NFL. 
• There is no first principle derivation. 
• Purely phenomenological, with a few exceptions.

 Now SS introduces the "Dictionary" in Duality. Given below.  There are a number of key ideas here, Quantities in D dimensions have their D+1 dimensional correspondence, eg T - energy momentum maps onto the metric tensor in D+1. There is also a mapping between the new dimension, z, and the RG flow, so that large z corresponds to low energy, small z to high energy.   There is also a boundary condition, so that the field j in the D+1 theory at the boundary z=0 is equal to the source term in the lower dimensional CFT. 

SS poses questions

Q- Can one explicitly construct hte gravitational theory form a a general QFT/quantum many body system? 

A- Yes we can!  One has to Quantize the beta function.   (Blogger: This is amazing - "third quantization"?! )

Here we go.  

Step 0 Write Z[J[x]] with sources Jn coupled to the fundamental ops On, such that any local operator allowed by symmetry can be written as a polynomail of the fundamental ops and their derivatives.  He gives the prescription for Ising, Vector and Matrix fields. 

Step 1  We need to do RG, keeping track of beta function for infinite many coupling constants. Let us simplify by removing the non-fundamental operators by introducing auxilliary fields. This is done with a delta function something linke

 jn (pn-On) - Jn pn + Jnm pn pm +....

jn is the Lagrange multiplier that enforces the constrain while pn is the dynamical operator.  

Step2  We integrate out the high energy modes of j. 

Q: why not j and p?
A: you can this, but lets see what we get by just integrating out the he j modes. 

If we do this, three things happen:

- By integrating out the quantum field, you generate energy that depends on the configuration of low energy j's and p's
- One obtains a quantum correction for the fundamental operators O.
- One also generates quadratic terms of the O's, which become p's.

Q: arent the fundamental fields the primary fields of CFT?
A: the fundamental fields are not the primary fields of CFT.  For example, they do not include spin...

Step 3 replace O by p. (Really the same as step 1).

Step 4 repeat 2-3 again and again until one has got rid of the original field completely.  One has now a theory in terms of a set of dynamical sources and dynamical operators. The interation parameter, has  become (magically) an additional dimension, with a j(n) and p(n) at each stage. 

Q: always local?
A: no - one needs arbitrary derivatives - locality is not guaranteed.

Q: you have two indices, m and n.... Whats the guarantee that the rank of the operators will not increase?
A:  you had this infinite no of fields at the beginning. It only becomes useful if you can truncate in tersm of a finite no of variables.

Q: how are you guaranteed that the truncation works at all stages?
A: so far I have not truncated... yet....

So now  the iteration variable has become a continuous extra dimension (idea of Verlindes...) and somehow, if it works, what is left is local with a truncated set of variables.  He says that this is sofar, an exact change of variables. A d-dimensinoal Z cn be written as a d+1 functional integration for dynamical sources and operator fields. Its a general scheme, but for a general theory, the holographic description is not useful.  When all sysmmetry allowed ops are large - some large N limit of the original theory - the holographic theory becomes classical.  The holographic theory always includes gravity - the energy momentum tensor becomes a spin-2 source. 

Q: whats the simplest CMT for which this can be carried out as an engineer?
A: I think its the O(N) model - vector model. I will show you.

Astonishing observation: Useful to consider z as time, one has p d_z j, as if p and j are conjugate to each other. So I can view the problem as a quantum problem in one higher dimension.   The partition fn is a transition amplitude of a D-dimensional Quantum wavefunction. The Hamiltonian generates scale transformation for the dynamical couplings.  The Heisenebrg equation, is a quantum beta function. 

Conventional RG is in J_n space, 

dJ_nm/Dl = beta(Jn,Jnm....). 

This is a "classical RG trajectory".  There are no fluctuations in the RG flow. 

Quantum RG is holography.  In this, flow, only fundamental operators appear. The price you pay is that these operators are now dynamical, and one has to consider a sum over  RG trajectories.  The RG flow is governed by a quantum hamiltonian

dJn/dl = [H,Jn]

If the large N theory is classical, this becomes classical.

Local RG prescription, spacetime dependent coarse graining - Gamma(x)=Gamma Exp [-alpha[x]dz]

By construction, Z is independent of alpha(x,z). Choosing different RG schemes corresponds to a gauge choice. 

Q: how will a fixed point arise in this quantum approach?
A: if you find a saddle point solution, then the sp soln will have scale invariance. 

Q: how can you justify one of the phenomenological models in the 1/N expansion?
A: I hope, but it has not been worked out so far.

Q: Can you reproduce or disprove the recent result of Verlinde, that gravity can be understood as an entropy. 
A: Yes - if you integrate high energy mode, you generate an action by a kind of order from disorder - gravity  appears - non trivial action a kind of entropic, quantum source.

Blogger- what a beautiful talk.  The idea of quantum RG as a route to holography may be a revolution. Lets hope so, because we need one.













 

Rafael Fernandes

Interplay between superconductivity, magnetism and nematic/orbital order in the iron pnictides

Blogged by Andy Schofield and Kedar Damle 

Started with in introduction of spin-fluctuations and other degrees of freedom. We have heard much about cuprates and the Mott transision We will be looking at pnictides where we are dealing with band physics. But the bands are complex yet it simplifies to some q2d electron and hole pockets ( a theorist’s view): Hole pockets in the centre of the zone (circular) and elliptical electron pockets at the X points:

Question: What about experiements? Good agreement with LDA in terms of shape though not always the mass, but see ARPES data later.

1. Unconventional Superconductivity:

A review of BCS superconductivity with phonons: The Cooper instability set as an exercise! The problem of computing Tc from first principles is difficult because of the lack of ability to predict the Coulomb pseudopotential. Rafael now moves to the blackboard. Want compute the partition function and he introduces the action for the electron phonon interaction: in the path integral formalism with coherent states. Then we get the Nambu representation of the problem where the electrons are a spinorial like combination of particle and hole. Constructing the perturbation theory gives a Dyson equation for the self-energy - and an Ansatz for developing superconductivity has a self-energy with off-diagonal parts representing the energy gap, W. It has a new dispersion E and a quasiparticle renormalization Z. BCS gets obtained in the limit that Z=1, E=dispersion and W is the gap.
Question: What is the physics of this limit? Answer: it is the limit of weak coupling.
Question: Is BCS limit applicable away from weak coupling - like in cuprates? Answer: no - but see later.
Question: Could you better define weak-coupling in terms of the parameters you introduced? Yes - I can introduce lambda which is like g^2 x density of states. There is another factor (m/M) which is small - ratio of the electron mass to ionic mass - so we can neglect vertex corrections.

So - are the iron based superconductors electron-phonon coupled? One calculation claimed maximum from e-ph is 0.8K in the pnictides - so that looks unlikely. Now let us look at the symmetries of the possible superconducting state: Crystal Lattice (X) Rotations (R) Time-reversal (T) and U(1) gauge. We look at the Cooper pair wavefunction in systems with inversion symmetry: singlet must be s- or d-wave while the triplet could be p-wve or f-wave etc. We will restrict to tetragonal singlet states with no T-breaking. Looking in 2D we have some simple possibilities:
s-wave: A_1g: no nodes - or x^2+y^2 extended s-wave with line nodes that are not fixed to symmetry lines.
g-wave: A_2g:  state unchanged by 90 degree rotation, but nodes along every 45, 90, etc degree - 4 lines of nodes
d_x^2-y^2: B_1g: state unchanged by 180 degree rotation - nodes at 90, 180 - 2 line nodes
d_xy: B_2g: line nodes
Electron-electron repulsion tends to favour nodal superconductors and we will consider pairing fluctuations by spin-fluctuations (Berk and Schrieffer, PRL 1966). We revisit these calculations and change to spin-fluctuations from bosons. The electrons now couple to a vector field and the new inverse greens function of the boson is the spin-propagator discussed in Andy Schofield's quantum criticality tutorial.
Question: what about vertex corrections? I will come back to this.
The spin-density means that the sigma_z involving the density goes to the identity which changes a sign to make the interaction effectively look repulsive not attractive.
Vertex corrections: now instead of being a small term (m/M) the spin fluctuations are also from the electrons so we cannot use Migdal's theorem. 
Question: I worked in Migdal's lab - and the theorem does not work if you use bare variables? AVC answers: there is a critical value below which this approach still works. 
Question: are we here in 2D where the boson coupling might be a relevant operator? Answer it is always relevant and we going to develop a theory here.
When visualizing the interaction it is repulsive at short range but changes sign and oscillates etc - and the diagonals it is purely repulsive. So put the nodes along the diagonal lines.
More on this in the next lecture...

Good evening blog watchers---we're back for the second installment
of Rafael Fernandes's double-header on superconductivity, magnetism,
and nematic/orbital order in the iron pnictides.


In the last lecture, Rafael gave a sketch of Eliashberg theory of phonon-mediated superconductivity (conventional)
and introduced the symmetry analysis of the SC order parameter,
focusing on singlet superconductivity with no time reversal
symmetry breaking in 2 dimensions (see description of previous lecture)
and then asked:
 
Why would the gap have nodes when the gap helps gain energy?
 
And his answer was: repulsive interactions.
 
To see how that works, he took the example of interactions mediated by
spin fluctuations and repeated Eliashberg theory, this
time for an interaction which couples the electron spin density to antiferromagnetic spin fluctuations, and showed
how the final gap equation gets an additional minus sign.

This minus sign comes from
the fact that the antiferromagnetic spin fluctuations mediate
a bonafide repulsive interaction.

Now in the second lecture, he's promised to start with this repulsive
interaction and show us how it leads naturally to a gap function with nodes when we look for solutions to the gap equation. So here we go with the
ball by ball commentary, a la cricinfo, of Rafael's second innings...

To begin, Rafael notes that the effective interaction in real space is proportional to \chi(r).
The gap would like to vanish across diagonals to avoid unfavourable
part of \chi(r), and that is the origin of the diagonal nodes in the gap.
 
For the detailed analysis, it is better to go back to momentum space and think
in terms of different parts of the Fermi surface connected by Q (Q is \pi,0
or 0,\pi). 

Simplification:  We can assume
V_{k-k'} = \chi(Q) \delta_{k-k',Q}
since the  real interaction has a strong peak at Q.

So we take two Deltas, \Delta_1 and Delta_2, on the two pockets
that are connected by Q, and get a two by two system of coupled
BCS equations for \Delta_1 and \Delta_2. Further, we can linearize
the gap equations (near T_c) and get two solutions:
One solution has an eigenvector with same sign for \Delta_1 and \Delta_2
The other has a relative minus sign. 

The equal sign solution requires
*attractive* interactions---this is the s++ state of Kontani and Onari,
which would need *orbital* fluctuations to mediate attraction.
The solution s+-, with opposite relative sign, is the one picked
by repulsive interactions, since the repulsive interaction looks effectively
attractive for this eigenvector.

Question: What is the cutoff to use in the momentum sum in the BCS eqn?
Ans: Bands are very shallow, so size of the pockets is the appropriate cutoff

Question: What about Coulomb repulsion (local)?
Ans:  Can show that this state can survive with little reduction in T_c

With this sketch of the mechanism for superconductivity, Rafael switches
focus to magnetism in the normal state:

The ordering is along two equivalent wavevectors Q_1 = \pi,0
and Q_2=0,\pi.
 
First question to address is: How do we describe the magnetically ordered state?
With an itinerant description or a localized picture of local moments ordering?

To explain this, Rafael now digresses to an elementary discussion
of antiferromagnetism in the Mott insulating state of the Hubbard
model, and explains how virtual charge fluctuations give antiferromagnetic
exchange interactions between the local moments of the Mott insulator.
This is contrasted with the prototypical example of an itinerant magnet, a Stoner
ferromagnet: 
Polarizing a free Fermi gas costs kinetic energy.
But a polarized free fermi gas pays less Coulomb repulsion energy
when we turn on interactions. At some critical value of the
Coulomb repulsion, this leads to ferromagnetism. This critical
value of repulsion is inversely proportional to the DOS at the Fermi
energy (Stoner criterion). Generalizing to ordering at some
other wavevector, say Q, the Stoner criterion becomes:
When U_Q \chi_0(Q) >1, itinerant SDW state is favoured.
Further, \chi_0(Q), the non-interacting susceptibility, is enhanced
if there is nesting with nesting wavevector Q, so it
is easier to have SDW instabilities when there is nesting.

These are the two limiting ways of thinking about magnetism.
Even in simple magnets like Ni and Fe, *neither* picture
applies literally, and we have to just make do with whichever picture
is closer to reality.

After this digression, Rafael makes his main point:
The pnictides are metallic, so it makes sense to choose the itinerant
picture to describe magnetism, even if they have significant correlations.

Question: When there is nesting, doesn't a gap open and destroy the Fermi surface?
Ans: That only happens if there is perfect nesting. Here we are not
thinking of perfect nesting.
In the pnictides, Q_1 and Q_2 are actually approximate nesting wavevectors
that connect the hole and electron parts of the Fermi surface. This nesting
gradually goes away on doping. And that is when the magnetism
goes away too. So the itinerant picture seems to hang together all right.
Of course, since the nesting is imperfect, there is still a threshold interaction
without which we would not have the SDW.

With this background, Rafael moves on to a more detailed
theory for the itinerant magnetism, basically doing a Hertz-Millis
theory for two simultaneous SDW instabilities (along Q_1 and along
Q_2). The final punch-line (details went by too quickly for a
ball-by-ball account) is

F_mag = \frac{a}{2} (\vec{m}_1^2 +\vec{m}_2^2) +\frac{u}{4}
(\vec{m}_1^2 +\vec{m}_2^2)^2 - \frac{g}{4}(\vec{m}_1^2-\vec{m}_2^2)^2

From the details that went by too quickly, 
Rafael concludes:  g>0

This g>0 picks stripes along one or the other direction from the plethora
of states that minimize the g=0 free energy. And these are exactly
the states seen in experiment. This gives qualitative agreement.
But does it work quantitatively?
The answer seems to be yes(!)
[the details again went by a bit too quickly for this blogger]

Q: What happen when g gets very large?
Ans: First order transition. But g is never that large in
the pnictides, so we don't need to worry about this possibility.

With magnetism in the bag, Rafael now moves on to discuss nematicity
in the normal state (already mentioned in earlier talks this week).

 Basic observation: The structural transition in the pnictides closely follows
the SDW transition, being slightly above the SDW transition (at slightly
higher temperatures). 

In the orthorhombic phase (below the structural
transition), experiments see strong anisotropies that cannot be attributed
to lattice distortions alone: A very tiny uniaxial pressure (of order
mega, not giga pascals) immediately leads to a resistivity anisotropy.
Now, the maximum resistivity anisotropy is at finite doping and
almost 100% in magnitude, while the maximum orthorhombic distortion
is at zero doping and tiny by comparison. So there must be
something electronic about the symmetry breaking of tetragonal
symmetry, and the lattice follows in the wake of the electrons.
This is what people mean when they talk of electronic nematicity.

Question: Are these measurements (of resistivity anisotropy) done above or below the SDW transition?
Ans: Both above and below SDW transition. Of course, the anisotropy
is largest below the SDW transition, but it is very big even above the
SDW transition (in comparison with the orthorhombic distortion).

Take-II on nematic order, starting from F_mag:

Ordering at Q_1 and Q_2 are both equally favoured.
To pick one of them, system has to break O(3) spin symmetry
and break the Z_2 symmetry (the symmetry that says Q_1 and Q_2
are equivalent).

Are both these symmetries necessarily broken simultaneously?
No!
In fact, the discrete symmetry breaking is less susceptible
to fluctuations, and we can imagine that the Z_2 symmetry
breaks first without O(3) symmetry breaking. This state,
with Z_2 symmetry breaking but no O(3) symmetry breaking, is
to be identified with electronic nematicity above the SDW transition.

In this picture, the nematicity comes from the spin physics, and other
things follow because they are coupled to the spin physics.

To put some flesh on this, in the last part of the lecture, Rafael moves on to consider the role of spatial fluctuations in \vec{m}_1 and \vec{m}_2
starting with F_mag derived earlier:
 
To do this, we decouple both quartic terms (g and u)  by two
separate Hubbard Stratanovich fields. The HS field dual
to the g term is the nematic order parameter. Integrating
out \vec{m}_1 and \vec{m}_2, one gets an
action functional for the two HS fields---one of these, \phi,
is the nematic order parameter, and the other \psi, gives
the magnitude of the tendency to magnetic order.
Next, we look for the saddle point of this action.
The saddle-point condition gives two coupled equations
for \psi and \phi at the saddle point.

Punchline: \phi is non-zero at the saddle-point *without* any magnetic
order developing---this happens because of
terms in the action coming from magnetic fluctuations (which
we integrated out to get the action for the HS fields). This is the transition to the nematic.  In this picture, this nematic order parameter (in the spin physics)
then couples to orbital degrees of freedom and induces
orbital order and everything else follows.
This is a nice way to rationalize, if not actually explain, the essential
features of what is seen experimentally.

And this concludes Rafael's very nice overview of the theory
for pnictide superconductors.
 
 


 

Friday, 10th August,

Hai Hu Wen (Nanjing University, China)
Materials and pairing mechanism in iron pnictides/chalcogenides:  
what we have learned and have still to learn.

Blogged by Leni Bascones and Piers Coleman















Hai Hu will start presenting the FeAs and FeSe based materials and structures. He talks about the discovery of superconductivity at 26 K in doped LaOFeAs by Hosono's group. He calls attention to  the large resisitivity of this material and the resistivity anomaly which was observed and that was later known to be an spin density wave transition. He notes that many of the parent materials had been synthesized some time before but were not studied in detailed.  Quickly after the discovery of superconductity above 50 K was found in related materials of the same family, so called 1111. Later on superconductivity was discovered in other families, like 122 or 111, what also contained FeAs layers, and in 11 famlily with simple structure based in FeSe layers. Nowdays there are seven related  families showing superconducting. Superconductivity is also found in Ni-compounds.

In most cases parent materials are non-superconducting. Superconductivity can be induced by electron or hole doping, by non-dopant substitution or by the application of pressure. Parent materials show an antiferromagnetic instability . It was early proposed that antiferromagnetism was due to Fermi nesting. Later on a different interpretation in terms of local moments was put forward. Magnetic order is called stripe or co-linear and show antiferromagnetic order along one direction and ferromagnetic along the other direction. Through the phase diagram, plotted as a function of pressure, the superconducting critical temperature shows a dome shape. A similar phase diagram is found when doping with electrons or holes. Antiferromagnetism disappears and superconductivity shows up.

Hai Hu compares the phase diagram of iron superconductors with that of cuprates. Cuprates are single band antiferromagnetic Mott insulators . with an exchange constant of order 150 meV while pnictides are multi-band metallic materials with an estimated second nearest neighbor exchange constant of order 50 meV.
He focuses on the transition towards antiferromagnetism and presents experimental results which show that at temperatures slightly larger than the Neel temperature there is also an structural transition. The gap in temperatures between the  structural and Neel temperatures depends on the family. He says that there are  two main proposals to explain the structural transitions  one based in spin nematicity and the other one in orbital ordering. Andrey Chubukov points that so far there are no microscopic calculations to support the  orbital ordering proposal. Structural details like As height or Fe-As.Fe angle seem to determine the optimal superconductivity. Theoretical input on why this could happen was given by Kuroki et al in 2009.

Hai-Hu wonders whether nematicity is important for superconductivy or not and whether it is just a consequence of magnetic or orbital fluctuations. He talks about transport measurements in detwinned samples by I. R. Fisher group which showed resistivity anisotropy with conductivity larger in the antiferromagnetic direction. Anisotropy was observed even above the structural transition and it has been discussed in terms of nematicity. Rafael Fernandes points out that because strain is applied to detwin the samples, above the structural transition one cannot talk about symmetry breaking. Other experiments showing anisotropic features where  published by Davis's and L. Green's group. Recent experiments in Matsuda's group suggest that the nematicity starts at temperatures much higher than the structural transition.

Hai-Hu suggests to try all kinds all of possibilities to make new materials. In particular he suggests to try systems with FeB and FeGe layers. So far only Tc ~5K have  been achived in these compoung but he hopes that Tc could become larger. To try new possibilities for materials lead to the observation of superconductivity in hole doped 1111 compounds, oxygen free 1111 materials and in more complex FeAs based materials. More recently superconductivity was observed in KFe2Se2 this compound is heavily electron doped. Some related compounds show Fe vacancies and are antiferromagnetic insulators. This family is called 245. Two different superconducting phases have been found in this family as a function of pressure. Q: Rafael Fernandes asks whether superconductivity in this materials is a bulk property . A:Hai Hu notes that the superconducting volume in not very large. Q: Andrey Chubukov asks whether there is phase separation A: yes it seems so.   There are current efforts to avoid Fe vacancies.

He concludes the talk saying that there is still some space to be explored for making new superconductors.

Q:  About Sr4V2O6Fe2As2 at high magnetic fields, whether a 2D vortex pancakes has been observed. A: Not directly.
Q: Why is iron special? A: Because of a possible balance between correlations and Drude weight.
Hai-Hu believes that many other superconductors without Cu or Fe will be found
Q: About the mechanism of superconductivity. A: Phonons seem not to mediate superconductivity, which seems related .to antiferromagnetic or orbital fluctuations.
Some other questions were asked but I could not hear too well the participants from my place.



Part II

Well, we're off to the races again!  After a short break, Hai Hu is begining his second lecture. He mentions that in his opinion, the iron based superconductors are intermediate coupling in character -
lying between the two extremes of spin fluctuation theory and the RVB theory of superconductivity.  He writes down the BCS formula, noting that over regions where the interaction is strongly repulsive, the gap likes to have different signs. Since the strongest interaction is betwen the electron and hole pockets, this lead to the proposal(by Igor Mazin and others), that the order parameter must have s+- symmetry, changing sign between the electron and hole pockets, but without a node crossing the Fermi surfaces. Proving that this is the nature of the pairing proves to be difficult, he says, and we don't have much direct evidence for the change of sign of the OP at this stage, though we have lots of evidence for a fully gapped Fermi surface.

Measurement by ARPES, shows that there are in fact two gaps, a feature of multiband superconductivity.  (I was not sure which part has the largest gap - the electrons or the holes? ) 

Using Hall probes, it becomes possible to measure the superfluid density.  There is an interesting temperature dependence, which can be fit to a two-component form, in which rho_a and rho_b both have BCS temperature dependence, with gaps

Deltaa= 1.6 meV,  Delta_b = 9.2 meV

rho = x rho_a + (1-x) rho_b

with a fit value of x =

Now the Hall constant is also consistent with multi-band physics. The strong temperature dependnece of the Hall constant is said to be a consequence of the multi-band character. This is contraversial, and some interpret this as a strong correlation effect, as a result of temperature dependent Z. I prefer to keep the interpretation simple, he says.

Now Hai Hu turns to NMR measurements. He notes the relationship

1/T_1T ~ Sum A(q)^2 chi''(q,omega)/omega at \omega

at omega = 0.  The upturn in 1/(T1 T) is consistent with antiferromagnetic spin fluctuations.

Now RPA spin fluctuation theory is predicted to have a sharp peak  below Tc - a resonant peak that is indeed observed in experiments.  This is consistent with s+-.   A second  measurement is using Fourier transformed STM measurements, carried out by Haneguri et al.  The magnetic field enhances sign-changing scattering, and this is what is observed in Fe(Se,Te).  Unfortunately so far, we have been unable to reproduce this scattering.

Q: what about sc loop experiments with half flux by Tsui et al?
HHW: Unfortunately, this also has not been reproduced and I am very sceptical.

Now he turns to the debate on gap structure.  There is a table -


ARPES - sees isotropic gap

SUPERFLUID density - most time shows powerlaw dependence, evidence of nodal gap.

NMR low T  1/ T1T shows power law, consistent with nodal gap or the s+- under impurity scattering

THERMODYNAMICS : also shows specific heat consistent with nodal gap


Now the spin fluctuation models the iron pnictides are found to give rise to gap anisotropy, but ARPES has not see it.

Q: Isn't this apples and oranges, doesn't a gap anisotropy exist in the 111
A: yes - (but blogger didn't understand the details of the answer...)

Linear dependence of the superfluid density (from penetration depth) is consistent with line-nodes in some materials, but with full gap on other materials.  Now many samples have lambda ~ (T)^n, with n =2 . Not consistent with ARPES data.

Thermal conductivity in Ba(Fe(1-x)Ni_xAs)_2, for current along the c-axis, there is evidence for a node in this direction. Now in Ba(FeAs1-xPx)_2, there is evidence from four fold oscllation in the thermal conductivity, that there may be nodal lines in two directions (see figure below).  Yet Zhang et al on the same material have data consistent with a different gap assignment.

Hai Hu also sees a four-fold oscillation of the C/T in a field in Fe-Se. (see Nature Comm, 1, 157 (2010). This has been phenomenologically fitted by Vorontosv and Vekhter, PRL 105, 187003 (2010) and Chubukov and Eremin (reference not gotten).

Continuing the discussion about gap anisotropy, in the sf theory, intrapocket scattering will enhance gap symmetry.  This remains a very contraversial issue and many groups are working hard on this topic.

Quantum Critical Point:  Much circumstantial evidence for a hidden quantum critical point.

(1) Entropy S(T) ~ T ln T
(2) Resistivity rho(T)= rho_0 + AT^n, where n is found to go down to n=1 at x = 0.4, but rises towards n=2 either side.
(3) Penetration depth seen to have a divergence.

How strong is the pairing: do we have a pairing group?  In the K-doped BaFe2As2, the jump in C/T is about   100mJ/mol/K^2.  This is consistent with delta C/C_n ~ 2, like strong coupling.  Canfield gorup has found C/Tc ~ T_c^2,  which has been interpreted by different groups in different ways.
(impurities + s+- one group, quantum criticality another group).

STM -

Hai Hu talks about STM in BaK Fe2As2.  His group has seen a dip-hump structure in the STM measurements. Giving an Eliashberg style interpretation, they can read-off

Delta = 7.5meV
Omega = 14meV
Delt + Omega = 21.5 meV

Hai Hu compares with the classic electron-phonon example, Rowell et al, and others used d^2I/dV^2 to read off the phonon spectrum. This is the classic example from lead.  HHW compares the two -
On the left hand side, dI/dV,  x=1 corresponds to omega = gap + resonant frequency.  Now shows results for the irons.

Now compares with Eliashberg simulation, puts in a strong mode at 14.5meV, for inter-pocket scattering. Comparing the blue simulation with the red expt, the two look qualitatively similar. 
Similar calculations for cuprates,

To convince you that the 14meV mode is not phonons, we have done this on more than one material - now on NaFeCoAs- still see a wiggle feature similar to the 122. Gap energy 5meV, mode energy 7-8 meV, consistent with the neutron resonance feature. Putting them all together,  neutron resonance energy versus STM wiggle data, find that

mode energy/ Tc ~ 4.5

Emerging Challenges

(1) Why does superconductivity survive with enormous impurity centers.  ON site doping induces stron impurity scattering, but superconductivity survives.  25% doping still gives superconductivity.
This is not consistent with an Abrikosov-Gorkov theory of splusminus.  A glaring inconsistency!

Remark:  Pressure effect and doping effect give comparable Tcs, even though one adds disorder, one does.

Q: What happens if you dope zinc onto the Fe site.
HHW:  No effect, but maybe on overdoped side.

Further data - Co doped Ba122 has an enormous gamma, but Tc is not effected.
Further data,  Cu and Mn doping on the Fe site,  exactly smae Tc reduction.

Rafael - one of the difficulties is that we don't know how to model the detailed impurity potentials.
HHW - still very hard to understand - one should still get large momentum transfer.

Further data - STM shows that Co doping does not affect the DOS very much. One would expect an ingap state forming from cobalt, but not seen. Small scattering potential or small momentum transfer scattering?   (The blogger is very sceptical about all of this - it all sounds like adding epicycles!)

(2) KyFe2-ySe2

arXiv1012.5164 

Absence of hole pocket - yet still pairing. The absence of the pocket is different to DFT, and it is not seen in ARPES. My group found that these samples are not homogenious, a dip in the field dependent magnetization. Signs of phase separation. Big debate in china

(1) I think the sample is inhomgenious. Second phase K2Fe4Se5
(2) Many disagree.

But I think now we know that the sample is in homogenious. 

Just recently STM data  - white area is 245, only the grey area is the superconducting phase - islands? Perhaps consistent with small sc fraction.

But with this sample, K0.8Fe1.6 Se2 - Keimers group sees a resonance - which they suggest corresponds to coupling between 0,pi and pi,0 electron pockets.  This experiment claims to reconcile the basic picture based on the AF SF mediated pairing.

Q:  Why is the sc volume so small still see this feature in the neutron scattering. ?

(3) Drude Weight. Slide from Basov. If you want high Tc, need strong correlation, but mobile carriers.

Concluding remarks.
s+- model - support from many experiments. Multiband widely observed.

(2) In most vases, the gap is nodeless. While gap anisotropy should ne an event with high probbablity, whcih so far disagrees with ARPES>

(3) The weak coupling picture with the Splus minus can account for some results, but it is challenged by some recent expts - the pair breaking effect induced by nm disorder is weak and the missing of hole pockets in KyFe2-ySe2.

(4) QCP, electronic nematicity, orbital physics have been observed in some systems. It needs more efforts to resolve how they relate to superconductivity.




Q: Is there any evidence for superconducting fluctuations.
HHW:  They are weak. No Nernst effect like in the cuprates.

Q:  Given you have multi-band, you can have diversity of band structure, and then you probably don't need a node to fit the data.
HHW:  At low T, the small gap will still dominate, but we don't go to low enough temperature.

Andy Schofield (University of Birmingham, UK)

Quantum Criticality - A tutorial


Blogged by Michael Norman and Piers Coleman

Andy is going to do a blackboard talk so let's see how good my eyesight is.  The focus will be on ZrZn2, a weak ferromagnet, with the emphasis of how current-current interactions affect metals, and whether the standard Hertz-Millis theory (time dependent Ginzburg-Landau) works or not.

To motivate all of this, let us consider a few cases first.  The "strange metal" behavior of cuprates exhibits linear T resistivity over a wide range of temperatures, but the nature of the "ordered" (pseudogap) phase is controversial.  CePd2Si2 is an antiferromaget, which is suppressed to zero under pressure.  Near the resulting quantum critical point, one sees unconventional superconductivity.  Or consider a first order transition (like liquid-gas).  At the end of the first order line, one has a second order critical end point, which in principle could be tuned to zero by varying some quantity like field, pressure, or what have you.

Q: What do you mean by critical fluctuations?
AS:  Near the ordering phase line, small variations of the order parameter field lead to large responses.

In ZrZn2, the electrical resistivity varies as T^5/3.  The thermal resistivity instead varies as T.  This is seen in nickel doped palladium as well, where Ni doping drives paramagnetic Pd into a ferromagnetic state.  The phase line varies as (x-xc)^3/4, where xc is the concentration of Ni that first induces ferromagnetism.   In Ni doped Pd, the specific head coefficient C/T varies as the log of T.







Now to the tutorial.  In Landau theory, there is a one to one mapping between non-interacting electrons and fermionic quasiparticles.  One can characterize the system by a distribution function, n(E), which varies with momentum, k.  The difference from the Fermi function is determined by interactions.  This can be determined by a scattering rate, which can be calculated using Fermi's golden rule, taking into account the presence of a filled Fermi sea.  One finds that the scattering rate depends on omega^2, where omega is the energy loss.  Including temperature, omega^2 changes to omega^2 + (pi*T)^2.

This is a phase space argument.  Now, let's assume the scattering potential depends on momentum and energy.  Exploiting energy and momentum conservation, one sees that the transferred energy, omega, is restricted to being (T=0) between zero and the energy E of the state, whereas the transferred momentum is restricted to being between omega/vF and 2kF, where vF is the Fermi velocity and kF is the Fermi momentum.  The result for the scattering rate (easily derived by power counting) is

1/tau ~ Integral(0 to E) omega domega Integral (omega/vF to 2kF) q^(D-3) dq |V(q,omega)|^2 where V is the scattering potential and D the dimensionality.  If V is constant, in D=3, this gives E^2 as before, whereas in D=2, one gets E^2log(E) instead.

If V has structure, then one gets something more interesting.  Coulomb scattering looks promising, since V ~ 1/q^2, but screening converts this to 1/(q^2 + qTF^2) where qTF is the Thomas-Fermi wavevector, and the infrared divergence is cutoff.

On the other hand, magnetic scattering is not screened, so this is more promising.  Assuming an Amperean potential between currents, j.  Using Maxwell equations and Ohm's law, the current-current scattering potential varies as 1/(q^2 - omega^2/c^2 + i*omega*sigma) where sigma is the conductivity.  The last term in the denominator is the so-called skin effect.  In the clean limit, sigma varies as 1/q.  So V^2 goes as 1/q^4 down to q of order omega^(1/3).  The result is that 1/tau (D=3) now goes like E instead of E^2.  Since 1/tau is a measure of the imaginary part of the self-energy, by Kramers-Kronig, one can show that the real part of the self-energy goes as E*log(E).  Therefore, the specific heat coefficient goes as log(T).

But the problem is that the ratio of the Amperean potential to the Coulomb one goes as vF^2/c^2, which is of order 10^(-6).  So, although one does indeed find a breakdown of Fermi liquid theory, this only shows up at extremely low temperatures.

Q:  This looks like a classical treatment?
AS:  Yes and no.  One has a Fermi surface, and then treats things in a semi-classical approximation.

Part II.  Andy begins with a summary of the first lecture.  The blackboard is empty and we are ready for another wonderful blackboard talk. Andy is going to use the results from the last lecture to gain insight into the magnet quantum critical point.  Andy says - if I think about an electric current and imagine how it is affected by small angle scattering.  A quasiparticle receives a tiny knock, and is now diverted through a small angle - this contributes to the decay rate of the quasiparticle, but it does not affect the transport current very much. (Bloggers aside: We saw this yesterday in Lara Benfatto's talk - this is the effect of the vertex corrections. ) The change in the current is

Delta j = k_F (1-cos (theta)) ~ k_F * (q/k_F)^2

which is reduced by the factor q^2s, so that transport rate is now

current decay rate = Integral omega domega Integral  d^D-1 q dq/ q^2  * |V(q,omega)|^2

                                * additional q^2 term

The q^D-1 cancels with q^2 in D=3, the |V(q,omega)|^2 ~ 1/q^4 at q^2  > omega/q, so the lower limit becomes omega^1/3, so when we do it, we have dq/q^2 from omega^1/3 , which gives 1/omega^1/3 from the q-integral, which gives in the end, with the frequency integral omega^5/3 -> T^5/3. (Blogger's aside - this result is consistent with simple dimensional analysis! AS answers that it is good to see how this works in detail. )

Q: wouldn't you have to do this self-consistently, because the resistivity appears in the damping rate?
AS: Potentially - but it comes back to whether the effective mass should be calculated self-consistently.  But the answer seems to be, it doesn't affect anything.

AS asks - can we use these results for U(1) gauge theories, where the coupling constant is much bigger.  AS reminds us about the method that was used by Yong Baek in his talk on spin liquids -

  fermion  = spinon creation * holon                         (slave boson approach)

Now this introduces a local gauge invariance, and to make this work once the spinons are delocalized, you need a fictitious electromagnetism.

Q: Is this really fictitious - after all it leads to a collective " artificial light ",
AS: I wanted to make the point that it is not conventional Electromagnetism.  It is observable, because it will lead to  a T^2/3 specific heat.  Andy points out that the energy will go like
T^2/3. (Blogger didn't quite catch it all).


Now we discuss Matter close to quantum criticality.    The action is written down

S = phi[ r0 + q^2 + |omega|/Gamma(q)]phi + u phi^4

Why do I have a term proportional to omega?  Answer - because this is allowing for the physics of damping?

quasiparticle interacts with medium that is almost magnetic, and it sends out modes with a propagator that is the inverse of the quadratic coefficient of S

1 / [r0 + q^2 + |omega|/Gamma(q)]


If you were in an insulator, the damping would be replaced by omega^2.  But here we have a metallic environment, the magnon interacts with the Fermi sea which makes particle-hole pairs.

Q: can this be derived?
AS: Yes, but we now know there are some problems with the derivation (non-analytic terms in frequency for example).

So in a system like ZrZn_2 close to criticality, the propagator of the critical magnetization is essentially identical with the current-current fluctuations we talked about this morning, but with a much stronger coupling.  And we see a T^5/3 resistivity as expected. Note that the thermal resistivity,  which is just governed by the quasiparticle relaxation rate, is still linear in T, as measured by Smith et al in the data shown below.

Q: how do you derive this from the partition function?
AS: Well - we'd like to rewrite the Boltzmann partition function in terms of states that are not eigenstates? Fortunately for me that question was answered long-ago by Feynman, who wanted to use position eigenstates in zero temperature qm.  He showed that you could evalue the expectations of

<r | exp[-i H t] r'>

provided you split it up into tiny increments, and then sum over all "histories" {r(t)}.  I'm trying to do exactly the same thing here,

< phi | exp[- H beta] |phi> = Sum over the {phi_j} configurations of

               < phi | exp [ - H \delta \tau] |phi_1> x ..... x <phi_N-1| exp[-H \delta \tau |phi

I now have imaginary time, and I have to split it up into all trajectories of the magnetization in imaginary time.

Q:  I understand all of this, but why does it give rise to the precise form in S that you have shown us?
AS: The answer is that this is the first allowable term in the expansion - why do I have a q^2 - the first that is allowed - you might have though omega^2,  but because this is in a damped environment, you can have a |omega|.  Actually what we have here is the Lindhardt function - a polarization bubble which has precisely this form.

Q: But why do you have a 1/q in the damping omega/q.
AS: I kind of lied to you, because  ferromagnet is an eigenstate. But when we look at long wavelength modes, (draws a wave) . In the FM, the decay rates are suppressed as the wavelength gets longer and longer, and this gives rise to a damping rate Gamma(q) ~ q.  Balistic motion - the amount of time is proportional to the wavelength, which gives tau ~ lambda, 1/tau ~ q.  But if it was a dirty ferromagnet, the electrons would diffuse, so now tau ~ lambda ^2, 1/ tau ~ q^2. Final thing I should mention is an antiferromagnet.  Now it doesn't depend on the slight variations about the AFM wavelength, so damping rate is constant.

So for an antiferromagnet, the propagator becomes

1 / [ r0 + (Q-q)^2 + |omega|/Gamma_0]

where we expanding the Gamma around the afm wavevector.  So now I can change my scattering rate formula, which now becomes centered around Q.

 (Q-q) -> qtilde

The denominator has now gone away becomes big Q^2.  The q^2/k_F^2 disappears because the scattering is now at large Q, which relaxes the current easily.

Q: Why don't you change the lower limits of integration in momentum?
AS: The upper cutoff isn't really important. Its kind of order (k_F). The lower cutoff is now when p^2 ~ omega, so lower limit is indeed changed to omega^(1/2)


But why is all of this wrong?  

Well experimentally - in the FM - almost all of them become first order before we reach the QCP. (Bloggers aside, there is a new Yb system which does have a second order transition, but its more localized)

MnSi is a particularly fascinating case.  It also doesn't go quantum critical - weakly first order - and worst, the power law, which is not actually T^5/3, but T^3/2, appears over a wide range of the tuning parameter (presssure) - and nobody understands this.

Theoretical reappraisal. 

It turns out that there are additional terms in the LGW action. A more detailed analysis tells us that terms I've left out should affect the answer.  Finally - almost everything I've discussed now applies to itinerant systems, where the magnetism is delocalized, but a lot of the crucial experiments are on f-electron systems where the magnetism is very localized, and the itinerant approach I've described here doesn't apply.

A better job of dealing with the FM QCP, there are non-analytic terms, eg in 3D, q^3/2 terms, which leads to fourth order terms that go negative, explaining why the transitions tend to go first order.
The current picture of the FM QCP is as follows:


Now the electrons are coupling to the transverse modes. The early pioneers did not quite take into effect the higher order transverse modes - but if you can gap them out by applying a field, you do get interesting quantum criticality at a metamagnetic QCP.

Puzzles in Heavy Fermion QCP.

Examples include CeCu6-xAu_x

The reason we thought things were fine - that we can ignore the mode-mode coupling terms can be ignored (above the upper critical dimension) - yet there is evidence that the system obeys E/T scaling - a result of something called "naive scaling" -  which suggests that the underlying quantum critical point is somehow below its upper critical dimension.  There is other evidence that the critical fluctuations are affecting all the Fermi surface  - some kind of local quantum criticality.

Another example is YbRh2Si2, which has an incredibly low ordering temperature that is killed off by a tiny magnetic field. Seems to be an additional scale that is collapsing to zero T^* at the QCP. This is one of the great puzzles.

Ends with a cartoon about what might be going on. Conduction electron zooms past a spin and exchanges spin with it. The key question, is what is the fate of the localized spins. One side - the ordered state - they are localized - on the other hand, there is another possibility that the interaction between the electrons and the local moments could undergo a Kondo effect, whereby the electrons and local moments bind in delocalized heavy fermions.

An example of a delocalized heavy fermi liquid, Andy gives UPt3, where the volume of the FS includes the f-moments. The picture thats emerging, is that the QCP could be the merging of Kondo and magnetism - a direct competition between the formation of the heavy fermi liquid and the magnetism. Its not clear that the magnetism and the failure of the heavy fermi liquid need coincide - but they seem to in some systems.

I just want to mention the new interest from String Theory - but which you will hear about on Monday - what little I know - there is a famous conjecture that says that strongly interacting theories in one dimension have a duality with a gravity theory in one higher dimension.  The idea is that if you can solve for the motion of particles in a classical gravity theory in one higher dimension will give you the interacting physics of a QFT in the lower dimension.  We might all have to learn, or at least remind ourselves about general relativity....

Strongly interacting QFT in D dims  <-------> Classical general relativity in at least D+1 dimensions.

Q: Andrey - maybe you should mention the names of Hlubina and Rice
AS:  It turns out, that shown by Robert Hlublina and Rice,  that you shouldn't do the average over the Fermi surface of the scattering rate, but the scattering time. And when  you do this in the clean limit, you get the result that the Fermi liquid T^2 scattering rate dominates.  Achim Rosch has shown that in the dirty limit, one can account for non-Fermi liquid behavior at a dirty 2D afm quantum critical point.

Q: Are there any cases where the simple derivation works?
AS: yes is the answer.  My favourite is the quantum critical end point of Strontium Ruthenate.  Even though the PT to AFM is driven first order by applying a field, you can still at finite field where we get QCP.  Does it work there?  Well, there is evidence that still more interesting things happen around the quantum critical end-point.

Q: Can you give some simple insight why here you have to take more and more terms, why its failing here, as opposed to BCS theory, where things work out.
AS: BCS is a simple case where you don't have to include fluctuations.  Here the problem is that we normally make the assumption that theres a single low-lying mode - but when we deal with metallic systems, we've go other low lying degrees of freedom - could be various types - what we're not able to do is to handle consistently all these low lying modes together.  But as a corollary, if you do this in insulators, everything works beautifully.  There are cases where quantum criticality does work beautifully, but I was limiting myself to the case of metals, where there are problems.

AChubukov.  If I were to answer the question of self consistency. I would answer that formally you can do self-consistency - there is some self-consistency at least at zero level. (We now know there are more subtle problems at higher order - blogger aside - this is a reference to the recent work of Metilsky et al. )

Thursday, 9th August

Elena Bascones
(Instituto de Ciencia de Materiales de Madrid (ICMM), Spain )
Mott physics: from basic concepts to iron superconductors

Blogged by Michael Norman and Natasha Perkins (with a little help from the start by Piers Coleman)

Elena begins with an introduction to Mott Physics. Kinetic energy from hopping likes to delocalize electrons.  In the atomic limit, we have a Coulomb repulsion term U which raises the cost of charge fluctuations and suppresses double occupancy.  In a single band system with one electron per site (on average)  as we increase U, we expect a Mott transition to localized electrons, because double occupation is forbidden.

Delocalized electrons (U << t) ---> Mott Transition ---> Localized electrons (U >> t)

Likewise, starting from the insulating limit, we have an upper and lower Hubbard band, separated by an energy U, corresponding to electron removal (lower band) and electron addition (upper band). These bands will broaden as we turn on the hopping between sites, with a width W proportional to the hopping t. 

Q: Isn't it more subtle. As you move your hole, don't you scramble your antiferromagnetic order?
EB: I haven't yet talked about AFM order.  Mott insulators can exist without magnetic order - in principle, you don't need to have magnetic ordering (e.g. in frustrated or low dimensional systems).

Hopping lowers the kinetic energy, whereas double occupancy costs you an energy U.

Now, let's approach the problem from the metal.  There is a band with width W.  There are four states per site - empty, spin up, spin down, and double occupancy. The average interaction energy is thus U/4.  The kinetic energy (constant density of states) is -W/4.  Therefore, we expect a transition when U=W from metal to insulator.  This simple picture assumes that double occupancy has a step jump to zero at U=W.

A better approximation (Gutzwiller) is to have the double occupancy vary linearly with U.  The kinetic energy is raised, but the interaction energy is lowered, with the resulting total energy being lower, and the transition is moved to U=2W.  The quasiparticle residue steadily decreases in the metal, disappearing at U=2W (Brinkman-Rice transition).

The real situation lies in between, and can be captured by dynamical mean field theory (DMFT).  On the metal side, there are now three bands, lower Hubbard centered at -U/2, a metallic band centered at 0, and an upper Hubbard band centered at +U/2.

We now turn to magnetism at half filling.  An electron can virtually hop to a neighboring site if the spins are opposite, leading a a savings in energy of J = t2/U where t is the hopping.  This leads to a AF (Neel) state.

Now, what about multiple orbitals?  For d electrons, crystal field splitting leads to t2g and eg states.  This modifies the on-site energies.  The hopping now depends on the orbital index.  The interaction contains intra-orbital and inter-orbital pieces, as well as Hunds rule contributions that tend to align the spins of different orbitals.


The interaction contains terms proportional to U (intra-orbital), U' (inter-orbital, different spin) = U-2J, and U'-J (inter-orbital, same spin) where J is now the Hunds coupling.  If we take the limit that J goes to zero, the problem simplifies.  One can show that in the Gutzwiller approximation, the Mott transition occurs at NW, where N is the number of orbitals.  This is reflected in DMFT, where the bands widen with increasing N.
With N greater than 1, one can now have a Mott transition away from half filling unlike the N=1 case where the transition is confined to half filling.


Q: What fillings are allowed?
EB:  One must have an integer number of electrons per site for a Mott transition.


Now lets switch on the Hunds J.  The energy is lowered when the spins are aligned on a given site.  With increasing J, the Mott transition is moved to lower U at half filling.  The opposite occurs away from half filling for n (site occupancy) of 1.  This is due to two competing effects, J reducing the degeneracy, and J changing the interaction energy.  The net effect is that at half filling, J increases localization, whereas away from half filling for n=1, J promotes metallic behavior.  This is confirmed by DMFT simulations.

For cases where n is neither 1 or N, J typically promotes "bad metallic" behavior.  Take N=3.  According to DMFT, Mott behavior is promoted at n=3.  n=2 and 4 lead to low coherence temperatures ("bad" metal with "spin freezing").  More metallic behavior is found at n=1 and 5.

Q: How does Hunds coupling affect the Mott gap?
EB: For half filling, gap = U+(N-1)J.  Away from half filling, gap=U-3J.


Q:  What is the physical origin of J?
EB:  This comes from the dependence of the Coulomb interaction energy on spin and orbital indices.

Leni part II (Blogged by Natasha Perkins)

Non-equivalent bands.

Two  different transitions for two bands give a possibility for orbital selective Mott transition.

 First consider Hund=0.  Two bands are degenerate.  Because of degeneracy, large difference between bands is required for orbital selective MT (OSMT).

Now  Hund is non zero. Hund’s coupling decouples orbitals. With finite Hund’s coupling the metallic state does not benefit from the degeneracy. The  band with smaller bandwidth becomes insulating first. OSMT can be obtained also in case of 3 and 4 bands, and is also affected by Crystal field.  Leni shows two examples of OSMT in which it is clear how the quasiparticle (QP) weight varies with the ratio Hund/Coulomb.

Iron based SC.

During last years many Fe-based SC were discovered. These are multi-orbital systems. Leni shows the PD for Fe-based SC.

 Correlations in iron-based SC are probably weaker than in cuprates, but are still important. One can see from the experiment Lu et al (Nature 2008), that mass enhancement is  about 3. From Basov talk (optics), we also saw that correlations are weaker. Contrary to cuprates, parent Fe-compounds are not Mott insulators. Does this mean that they are not correlated?

We should include all 5 orbitals to explain Fe-based SC. These 5 orbitals are different, there are 6 electrons on 5 orbitals, so we are not at half-feeling.  We can think about pnictides as about doped Mott insulator.

Iron SC are Hund’s metals. Correlations are enhanced by Hund’s coupling. This is possible because of the multiorbital character, which plays an important role – we can have coexistence of localized and itinerant electrons.  Leni shows PD from which we can see that correlated metallic state appears due to Hund’s coupling. Different Fe  compound are either more or less correlated.

Leni compares results from 2- and 5-bands model.

Liebsch(2010) also shows that hole-doping increases correlations.  Doping with electrons decreases correlations.

Andrey: the  PD is at T=0. Then what the words FL mean? Leni: Yes, it is T=0 because Liebsch is doing exact diagonalization.  ( I did not get Leni’s answer).

BeFe2As2 – PD with FL and NFL. Crossover T is governed by Hund’s coupling. NFL is seen when we are moving towards half-filling. There the QP weight is much smaller.

Rafael: You  expect that 3d5 will be insulating? Leni: Yes. Rafael: but if you dope  3d5 with electrons it becomes metal as other pnictides.  Leni and Rafael  discuss resistivity in different compounds.

Orbital differentiation in iron SC – degree of correlation is orbital depend. ( plot of QP weight for different orbitals). XY orbital has lowest QP weight.

Do we expect an OSMT in pnictides? XY orbital is the most correlated. In the plot we can see that in some materials the orbital differentiation is significant and in then we can expect OSMT, for example, in FeSe. OSMT is induced by hole-doping in FeSe ( results of M. Capone).

Andrey: Is it known where the spectral weight goes? Leni: there is a spread of spectral weight. Andrey: there are ARPES experiments which are interpreted as OSMT.  I want to relate your talk to Andy’s  talk this morning. What is about the frequency dependence of Z-factor? Does it change? Leni: I do not know such calculations.

Summary: one can have weak correlation due to U but still be correlated due to Hund.

How correlated are electrons? Which is the nature of magnetism in pnictides?

Let us discuss it in a more general sense. Magnetism can come even from weak correlations, Fermi surface instabilities, renormalized FL behavior. And of course, from simply localized picture, for example, from J1-J2 model which has been proposed to explain the magnetism in Fe-compounds ( stripes).

I am going to discuss first metallic AFM state (details in Rafael‘s talk). Columnar state with ( pi,0) ordering. Local-moment description – Heisenberg J1-J2 model. In this case the exchange appears from the second order perturbation theory, as in Mott state. J2 is rather large in pnictides due to hopping through arsenic ion. It has been proposed that J2>J1/2. There columnar order is stabilized.

 We computed J1 and J2. We showed that at small Hund,  the state is not columnar, but instead Neel state with (pi,pi). However, at large Hund, we can get columnar order with (pi,0). In fact, the orbital states in (pi,pi) and (pi,0) phases are not the same. There is of course a crystal field sensitivity of the orbital state.

Also, what one can get from localized picture is electron-hole doping asymmetry. We see that hole and electrons are going to different orbitals. Electron doping has a tendency to FM compared with n=6 parent compound ( LaOCoAs).

Andrey: in J1j2- the way how you select (pi,0) is due to quantum fluctuations. Is it also present in your analysis? Leni: no, these are higher order terms. It is probably quite complicated, one need to have bi-quadratic  exchange. We do Hartree-Fock.

Leni discusses Hartree-Fock PD, in which one can see (pi,pi)-( pi,0) transition with increasing Hund’s coupling.

YBK: Do you include orbital fluctuations?  Leni: yes, this is included. YBK: I have impression that you consider different orbital configuration and then compute exchange. Leni: Yes. YBK: But then you consider rigid orbital configurations, without fluctuations? Leni: This is the leading term.

What is the nature of (pi,0) state?

We focus on this state and try to understand what’s going on in this state. Leni shows the PD in parameter’s space of J/U  vs U. They have found three different regions: Itinerant phase with strong orbital differentiation, Non-magnetic insulating and Magnetic insulating phases. In itinerant phase not all orbitals are itinerant:  while xy and yz orbitals are gapped and insulating, zx, 3z^2-r^2 and x^2-y^2 are itinerant orbitals but with correlation features. It is interesting to see how one can go from one phase to another by doping.

Summary: multiorbital physics is important. Orbital differentiation is important and we should play attention to them.

Rafael: I have small issue about LDA+DMFT. There is a double counting of correlations in LDA and DMFT.

Leni: I din’t do this, but I know that people try to take this into account. We are working with tight-binding.  But the point is that different methods give similar results.

Gabovich: what is your opinion are about magnetic correlations?  Do they support SC?

Leni: I did not work on this issue, but I think in these systems fluctuations would support it.