Itinerant Ferromagnetism in a polarized two-component Fermi gas

Itinerant Ferromagnetism in a polarized two-component Fermi gas

Pietro Massignan ICFO - The Institute of Photonic Sciences - 08860 Castelldefels, Barcelona, Spain    Zhenhua Yu Institute for Advanced Study, Tsinghua University, Beijing 100084, China    Georg M. Bruun Department of Physics and Astronomy, University of Aarhus, Ny Munkegade, DK-8000 Aarhus C, Denmark
July 12, 2019

We analyze when a repulsively interacting two-component Fermi gas becomes thermodynamically unstable against phase separation. We focus on the strongly polarised limit where the free energy of the homogeneous mixture can be calculated accurately in terms of well-defined quasiparticles, the repulsive polarons. Phase diagrams as a function of polarisation, temperature, mass imbalance, and repulsive polaron energy, as well as scattering length and range parameter are provided. We show that the lifetime of the repulsive polaron increases significantly with the interaction range and the mass of the minority atoms, raising the prospects of detecting the transition to the elusive itinerant ferromagnetic state with ultracold atoms.

A mixture of two species of fermions with short range strongly repulsive interactions was predicted long ago by E. Stoner to display a transition to an itinerant ferromagnetic state Stoner1933 (). In analogy with immiscible classical fluids, the two components spatially separate to minimise their interaction energy. This strong coupling effect is notoriously difficult to analyze, and the conditions for the existence of itinerant ferromagnetism are still controversial. For instance, one can rigorously exclude ferromagnetism in one dimension Lieb1962 (), whereas it has been shown to exist in specific types of Hubbard models Nagaoka1966 (); Mielke1991a (); Mielke1991b (); Mielke1992 (); Tasaki1992 (); Tasaki1995 (). First order transitions to a ferromagnetic state have been observed in metallic systems as predicted by effective theories Belitz2012 (). However, the inevitable presence of disorder and of intricate band structures in solid state systems imposes great difficulty when comparing microscopic theories with experiments, and it is still debated whether a homogenous electron system becomes ferromagnetic at all.

An exciting new setting to investigate itinerant ferromagnetism is provided by quantum gases, which offer a precise determination of physical parameters and a great tunability Giorgini2008 (). Conditions for itinerant ferromagnetism have been derived in the cold atom context using mean-field, diagrammatic, Jastrow-Slater, and Monte-Carlo calculations Duine2005 (); LeBlanc2009 (); Conduit2009 (); Pilati2010 (); Cui2010 (); Massignan2011 (); Chang2011 (); Heiselberg2011 (); Palestini2012 (); Cui2012 (); deSaavedra2012 (); Sodemann2012 (); He2012 (). A recent experiment claimed the observation of itinerant ferromagnetism in a Li mixture Jo2009 (). Current consensus however is that fast decay to a lower lying attractive state precluded the realization of ferromagnetism in this experiment Pekker2011 (); Pekker2011bis (); Zhang2011 (); Massignan2011 (); Sanner2012 (); Sodemann2012 (). Such decay is peculiar to quantum gases as the repulsive states obtained by Feshbach resonances are always accompanied by a number of attractive ones.

A major step in the quest to obtain long-lived repulsive Fermi gases is the production of a Li-K mixture around a moderately narrow Feshbach resonance, which leads to a much smaller decay rate of the mixture Kohstall2012 (). This result raises the hope of observing itinerant ferromagnetism in quantum gases at Feshbach resonances which are not broad.

In this letter, we examine the conditions for the existence of itinerant ferromagnetism for a two-component Fermi gas consisting of -fermions with mass and -fermions with mass in a volume . The key point of our paper is that we focus on the limit of strong polarisation taking . An important result emerging from recent cold atom investigations is that it is possible to develop a quantitatively accurate description of the properties of the gas in this limit, in terms of well-defined quasiparticles. The quasiparticles consist of 2-atoms dressed by multiple excitations of the bath of 1-atoms. The relevant quasiparticle spectrum as a function of the scattering length of the atom-atom interaction is shown in the inset of Fig. 1. The spectrum contains a “repulsive branch” at positive energy, populated by quasiparticles known as repulsive polarons. There is also an “attractive” branch at negative energy and the corresponding quasiparticles are called attractive polarons. In addition, there is a continuum of states (grey shaded region in the inset of Fig. 1a) corresponding to molecules and holes with momenta Kohstall2012 () (or trimers plus two holes for light impurities Mathy2011 ()). Recent investigations showed that the polaron properties can be calculated with surprising accuracy in terms of microscopic parameters Combescot2007 (); Prokofev2008 (); Combescot2008 (); Chevy2010 (); Cui2010 (); Massignan2011 (); Mathy2011 (); Massignan2012 (); Vlietinck2013 (). It is the presence of a repulsive branch which opens the possibility to study repulsively-interacting systems with cold gases.

We derive the free energy of the homogeneous mixture in terms of the repulsive polaron energy and analyze when the homogeneous mixture becomes unstable against phase separation. Phase diagrams are obtained as a function of polarisation, temperature, mass-imbalance and polaron energy as well as scattering length and range parameter. We show that the lifetime of the polarons increases significantly with the range parameter of the interaction. This increase in the lifetime provides a much longer time-window for experiments, suggesting that itinerant ferromagnetism might finally be unambiguously detected with cold atoms.

We take the interaction between the 1- and 2-atoms to be strong and repulsive, and the intra-species interaction to be negligible. For a highly polarised mixture with , an accurate many-body theory describes the mixture as an ideal gas of -atoms coexisting with an ideal gas of repulsive polarons Pilati2010 (); Cui2010 (). In this limit, the free energy per particle reads


where is the free energy per particle of an ideal gas of -atoms with mass and density at temperature , and is the polylogarithm. The fugacity , with the chemical potential, is determined by where is the thermal de Broglie wavelength. is the energy of a zero-momentum repulsive polaron embedded in a Fermi sea of -atoms with density and Fermi energy , with . The factor in Eq. (1) is a rescaling of the polaron energy taking into account the fact that the impurities are immersed in a Fermi sea with density . In the weak coupling limit , the polaron energy is given by with . The strong coupling expression for is given in the Supplemental Material. Since we focus on the low- regime, we have neglected the temperature dependence of the polaron energy which is approximated by its value. The effective mass of the repulsive polaron is close to  Massignan2011 (); Massignan2012 (), and we have taken for simplicity. Quantum Monte-Carlo (QMC) calculations Pilati2010 () indicate that the expression (1) is accurate for polarizations (i.e., ).

The thermodynamically unstable region of the homogeneous mixed phase can be determined by applying the usual Maxwell construction to the free energy . Let us first focus on the case of equal masses . The case of will be treated later. For equal masses, one has . If given by (1), applicable in the regime , exhibits a minimum at , the homogeneous mixed phase become thermodynamically unstable when .

Figure 1: Phase diagrams in terms of the polaron energy , the polarization , and the temperature . The gas is mixed above the lines, and phase separated below. The inset shows the spectrum of a K impurity in aLi Fermi gas with , as in the experiment of Ref. Kohstall2012 (): visible are the repulsive and attractive polarons (red and green lines), and the molecule-hole continuum (grey shaded region), arising from holes and molecules with momenta .

In Fig. 1, we plot the phase diagrams obtained from a Maxwell construction using Eq. (1) as a function of the polaron energy , the polarisation , and the temperature . We have only shown the diagram for , where our theory can be expected to be accurate. For and , Fig. 1 shows that the system phase separates when . This reflects that the -atoms cannot diffuse into a polaron state in the ideal gas of -atoms if the polaron energy is higher than the Fermi energy. For smaller , phase separation occurs at a smaller polaron energy since the system can separate into two partially polarised phases, which reduces the kinetic energy cost. Conversely, we see that phase separation is suppressed at higher temperatures due to the entropy of mixing. Note that the phase diagram in Fig. 1 is generic since it is based only on the existence of well-defined and long-lived quasiparticles with energy , an assumption verified experimentally in Ref. Kohstall2012 ().

We now turn to study the effects of unequal masses . For simplicity, we consider and the limit (). A sufficient condition for the instability of the homogeneous mixed state can be found by comparing its energy with that of a fully phase separated state, where the 1-atoms occupy a volume and the impurities occupy a volume . Equating the pressures of the two fully separated phases, and using for an ideal Fermi gas, we find and . To first order in , the energy per particle of the fully phase separated state becomes


which is accurate when . To the same order in , from Eq. (1), the energy per particle of the homogeneous mixed state at is


The homogeneous mixture is unstable when which gives Massignan2011 ()


This result indicates that for fixed , phase separation is favored for heavy atomic species due to the suppression of the Fermi pressures. This effect was also discussed in Refs. vonKeyserlingk2011 (); Cui2012 (). An analysis of the ferromagnetic transition by the virial expansion, valid at high temperatures, is presented in the Supplemental Material.

In quantum gases, while the interaction potential is generally attractive, effective repulsive interactions can be obtained by preparing the -atoms on the repulsive branch of the Feshbach resonance depicted in the inset of Fig. 1 Jo2009 (); Kohstall2012 (). The effective inter-species interaction can be characterised by the -wave scattering length and the range parameter , where is the background scattering length, is the differential magnetic moment, and the magnetic width of the Feshbach resonance Petrov2004 (); Bruun2005 (). At the many-body level, a small/large corresponds to a wide/narrow Feshbach resonance.

To make a direct connection with experiments, it is useful to express in terms of the physical parameters and . A very attractive feature of the high polarization limit is that it is possible to calculate precisely even for strong interactions. The explicit expression of , obtained through a many-body calculation including one-particle-hole excitations from the Fermi sea of the majority atoms, has been derived and discussed in detail in Refs. Cui2010 (); Massignan2011 (); Kohstall2012 (); Massignan2012 (), and is reported for completeness in the Supplemental Material.

Figure 2: Phase diagram for equal masses for (thick solid lines), and (thick dashed lines). The gas is mixed above the lines, and phase separated below. The thin lines are the phase boundaries obtained from the perturbative expression (5) retaining terms up to , , and order. The green markers indicate the IFM transition at as found by Quantum Monte-Carlo calculations Pilati2010 (), second order diagrammatic theory Duine2005 (), and Stoner Stoner1933 () for and respectively.

We show the resulting phase diagram for equal masses in terms of the scattering parameters in Fig. 2 for two different values of the range: describing a wide Feshbach resonance, and similar to the moderately narrow Feshbach resonance of the experiment in Ref. Kohstall2012 (). We observe that a non-zero effective range shifts the phase separated region toward the BCS-regime (the right side of the plot), consistent with a similar shift of the polaron energy reported in Ref. Kohstall2012 (). As in Fig. 1, we have drawn the phase boundary lines only within the regime of validity of the polaron theory, i.e., . With increasing , we have furthermore terminated the lines where the polaron Ansatz fails due to decay as will be discussed in more detail below. For comparison, in Fig. 2, we also mark the critical values for the ferromagnetic transition calculated by various zero-temperature theories. The perturbative results shown in the figure are obtained by inserting in Eq. (1) the analytic expansion for the energy of a single impurity in a Fermi gas with hard-spheres interaction Bishop1973 (),


truncated respectively to , , and order. Note that these perturbative results should be taken with caution in the regime . It is also known that the third order term in the expansion is non-universal. It is interesting that Eq. (1) combined with the single impurity expression (5) to order in yields at essentially the same critical point as the order diagrammatic theory presented in Ref. Duine2005 ().

Due to the symmetry of the phase diagram for equal masses, the phase boundary must cross the axis vertically. As can be seen from Fig. 2, this restricts the range of possible extrapolations of our theory from its range of validity to smaller values of . In particular, the extrapolation to predicts a critical value for ferromagnetism inbetween the Monte-Carlo result and the mean-field result. Our theory also predicts a larger critical value of than the QMC result for . This is because the repulsive polaron energy obtained by our method is lower than the one found by QMC Massignan2011 (); Pilati2010 (), which is compatible with QMC being only an upper bound. Also, it could be due to higher order particle-hole processes omitted in our analysis.

Our thermodynamical analysis above is based on the assumption that the repulsive polaron is a long-lived excitation. However, the repulsive polaron state inevitably experiences decay into the lower branches, i.e., the attractive polaron state or one with molecules or trimers formed (cf. inset of Fig. 1a). It is therefore important to address the question: does the repulsive polaron state have a sufficiently long lifetime in the vicinity of the phase transition such that the experimental observation of the transition becomes possible? This question has been considered for the balanced and polarized cases respectively in Refs. Pekker2011 (); Pekker2011bis (); Zhang2011 (); Sanner2012 (), and Massignan2011 (); Sodemann2012 (). To take into account effects coming from a large in the strongly-polarized regime, we calculate the decay rate of the repulsive polaron state due to the dominant two-body processes by using a diagrammatic method (see Suppl. Mat. for details) which proved in very good agreement with the experimental data Kohstall2012 (). We find that for fixed range parameter, the decay rate increases with increasing repulsion, and eventually the repulsive polaron state becomes ill-defined due to fast decay as observed experimentally Kohstall2012 (). For this reason, at strong coupling we have terminated the lines in Fig. 2 when . However, most likely an even smaller decay is needed for the experimental observation of the ferromagnetic state. We now discuss how the latter may be achieved.

We plot in Fig. 3 the critical value of the interaction parameter for phase separation at and for different mass ratios obtained from (4), and in Fig. 4 the corresponding decay rate of the repulsive polaron at the critical coupling strength. Figure 4 shows an important result: a resonance with gives rise to much longer lifetimes than a broad one with . Furthermore, we find that a large mass ratio decreases the decay rate significantly compared to the case of equal masses. For instance, for a mixture of a small number of K atoms in a gas of Li atoms, the polaron lifetime increases by a factor at the critical coupling strength for phase separation when the range of the atom-atom interaction is instead of zero. By choosing appropriate mass ratios and using moderately narrow Feshbach resonances, one can suppress the decay rate of the mixed phase to .

Figure 3: Critical coupling strength for phase separation at and as a function of . Lines are for mass ratios 1 (solid), 40/6(dotted), and 6/40 (dashed). The circle and the square indicate the values relevant for the experimental conditions of, respectively, Refs. Jo2009 () and Kohstall2012 ().
Figure 4: Decay rate of repulsive polarons at the transition with and . Lines and symbols as in Fig. 3.

An unambiguous experimental signature of the itinerant ferromagnetism transition would be the observation of magnetic domains when the mixed gas is brought across the phase boundary. Domain formation was not detected in previous experiments Sanner2012 (), probably due to the fast decay with rate suffered by the atomic gas. The much slower decay of the repulsive polaron state predicted in this work when the range is significant can provide a ten-fold wider time window for measuring the signatures of the transition, during which notable domains may form and be detected. An estimation of the domain formation rate and size, though a worthy calculation, is out of the scope of the present paper. The instability towards domain formation may also be detected by measuring a sharp increase of spin fluctuations. Experimentally, one can now measure spin fluctuations with m-spatial resolution Meineke2012 () which indicates that this method might be very effective. An alternative method for detection is to prepare the gas directly in the phase separated state, and check its stability against mixing.

To conclude, we derived detailed phase diagrams of a two component Fermi gas in the limit of strong polarisation, where the effects of the interactions can be accurately described in terms of well-defined quasiparticles, the repulsive polarons. The phase diagrams were then expressed in terms of the scattering length and range parameter using a many-body theory known to be reliable in the strongly polarised limit. The ferromagnetic region was shown to move towards the BCS side with increasing range of the interaction. Finally, we found that a large range and impurity mass increase substantially the polaron lifetime, raising hopes for the observation of itinerant ferromagnetism in a quantum gas.

Note added – Recently, we became aware of related studies vonKeyserlingk2013 () which have appeared after submission of the present Letter.

Acknowledgements – It is our pleasure to thank M. Zaccanti, T.-L. Ho and M. Lewenstein for insightful discussions. This research has been funded through ERC Advanced Grant QUAGATUA, Spanish project TOQATA, Tsinghua University Initiative Scientific Research Program, NSFC under Grants 11104157 and 11204152, the Carlsberg Foundation and the ESF POLATOM network.


  • (1) E. Stoner, Philos. Mag. 15, 1018 (1933).
  • (2) E. Lieb and D. Mattis, Phys. Rev. 125, 164 (1962).
  • (3) Y. Nagaoka, Phys. Rev. 147, 392 (1966).
  • (4) A. Mielke, Journal of Physics A: Mathematical and General 24, L73 (1991).
  • (5) A. Mielke, Journal of Physics A: Mathematical and General 24, 3311 (1991).
  • (6) A. Mielke, Journal of Physics A: Mathematical and General 25, 4335 (1992).
  • (7) H. Tasaki, Phys. Rev. Lett. 69, 1608 (1992).
  • (8) H. Tasaki, Phys. Rev. Lett. 75, 4678 (1995).
  • (9) D. Belitz and T. R. Kirkpatrick, arXiv:1204.0873 (2012).
  • (10) S. Giorgini, L. P. Pitaevskii, and S. Stringari, Rev. Mod. Phys. 80, 1215 (2008).
  • (11) R. A. Duine and A. H. MacDonald, Phys. Rev. Lett. 95, 230403 (2005).
  • (12) L. J. LeBlanc, J. H. Thywissen, A. A. Burkov, and A. Paramekanti, Phys. Rev. A 80, 013607 (2009).
  • (13) G. J. Conduit, A. G. Green, and B. D. Simons, Phys. Rev. Lett. 103, 207201 (2009).
  • (14) S. Pilati, G. Bertaina, S. Giorgini, and M. Troyer, Phys. Rev. Lett. 105, 030405 (2010).
  • (15) X. Cui and H. Zhai, Phys. Rev. A 81, 041602 (2010).
  • (16) P. Massignan and G. M. Bruun, EPJD 65, 83 (2011).
  • (17) S.-Y. Chang, M. Randeria, and N. Trivedi, Proc. Nat. Acad. Sci. 108, 51 (2011).
  • (18) H. Heiselberg, Phys. Rev. A 83, 053635 (2011).
  • (19) F. Palestini, P. Pieri, and G. C. Strinati, Phys. Rev. Lett. 108, 080401 (2012).
  • (20) X. Cui and T.-L. Ho, Phys. Rev. Lett. 110, 165302 (2013).
  • (21) F. Arias de Saavedra, F. Mazzanti, J. Boronat, and A. Polls, Phys. Rev. A 85, 033615 (2012).
  • (22) I. Sodemann, D. A. Pesin, and A. H. MacDonald, Phys. Rev. A 85, 033628 (2012).
  • (23) L. He and X.-G. Huang, Phys. Rev. A 85, 043624 (2012).
  • (24) G.-B. Jo et al., Science 325, 1521 (2009).
  • (25) D. Pekker et al., Phys. Rev. Lett. 106, 050402 (2011).
  • (26) D. Pekker and E. Demler, Lecture Notes of the Les Houches Summer School, Volume 94 (2012).
  • (27) S. Zhang and T.-L. Ho, New Journal of Physics 13, 055003 (2011).
  • (28) C. Sanner et al., Phys. Rev. Lett. 108, 240404 (2012).
  • (29) C. Kohstall et al., Nature 485, 615 (2012).
  • (30) C. J. M. Mathy, M. M. Parish, and D. A. Huse, Phys. Rev. Lett. 106, 166404 (2011).
  • (31) R. Combescot, A. Recati, C. Lobo, and F. Chevy, Phys. Rev. Lett. 98, 180402 (2007).
  • (32) N. Prokof’ev and B. Svistunov, Phys. Rev. B 77, 020408 (2008).
  • (33) R. Combescot and S. Giraud, Phys. Rev. Lett. 101, 050404 (2008).
  • (34) F. Chevy and C. Mora, Reports on Progress in Physics 73, 112401 (2010).
  • (35) P. Massignan, Europhys. Lett. 98, 10012 (2012).
  • (36) J. Vlietinck, J. Ryckebusch, and K. Van Houcke, Phys. Rev. B 87, 115133 (2013).
  • (37) C. W. von Keyserlingk and G. J. Conduit, Phys. Rev. A 83, 053625 (2011).
  • (38) D. S. Petrov, Phys. Rev. Lett. 93, 143201 (2004).
  • (39) G. M. Bruun, A. D. Jackson, and E. E. Kolomeitsev, Phys. Rev. A 71, 052713 (2005).
  • (40) R. Bishop, Annals of Physics 78, 391 (1973).
  • (41) J. Meineke et al., Nature Physics 8, 454 (2012).
  • (42) C. W. von Keyserlingk and G. J. Conduit, Phys. Rev. B 87, 184424 (2013).
  • (43) K. Huang, Statistical Mechanics, 2 ed. (John Wiley & Sons, New York, 1987).

Appendix A Supplemental material

a.1 Energy and decay rates of the repulsive polaron

The quasiparticle properties of a polaron, i.e., a single impurity (2-atom) dressed by interactions with a Fermi sea of 1-atoms, can be derived from the knowledge of the impurity self-energy , which within the 1-particle-hole approximation and at zero temperature reads Chevy2010 ()


with the kinetic energy measured from the chemical potential (we have set ).

The T-matrix for two-particle scattering reads Bruun2005 ()


with the energy in the center of mass reference frame of the scattering two particles, , and the renormalized pair propagator


The polaron energies at zero momentum are determined by the equation , which generally has a negative solution , corresponding to the attractive polaron, and a positive solution , corresponding to the repulsive one. The corresponding residues are given by .

In the leading decay process, a repulsive polaron decays into an attractive polaron by scattering a majority particle out of the Fermi sea Massignan2011 (); Kohstall2012 (). To describe this 2-body decay channel, we use the fact that the impurity Green’s function can be approximated as


close to its poles , with the effective mass of the polarons. Replacing the bare impurity Green’s function with inside the pair propagator Eq. (8),


and using in Eqs. (6) and (7), the decay rate of repulsive polarons to attractive ones is given by


For simplicity, in the calculation we have approximated with the bare value .

a.2 Virial expansion

In the high temperature regime, we examine the itinerant ferromagnetic transition by the virial expansion. To second order, this expansion gives for the partition function of the two-component Fermi gas


with . When only the -wave “upper branch” of excitations is taken into account, the second virial coefficient is Huang1987 ()


The -wave phase shift is given by . At a broad resonance one has , whose minimum value is at . For a very narrow resonance, we find at the unitary point. Here .

The free energy per particle of the mixture is


where we have used obtained from (12). The phase diagram will have a phase separated region when


for some values of , which is possible only if . For equal masses, the region of phase separation derived from the Maxwell construction is bounded by the concentrations which minimise , i.e.,


The phase diagram obtained from (16) is plotted in Fig. 5 for and . Since there is no kinetic energy cost of phase separation for high temperatures, this phase diagram is a result of the competition between the repulsive interaction energy and the entropy of mixing. The predicted critical temperature for phase separation unfortunately is too low for the virial expansion to be reliable. Indeed, the largest transition temperature is obtained at unitarity for a broad resonance where . The calculation nevertheless indicates that a large range decreases the critical temperature for phase separation, consistently with the low temperature polaron calculation.

Figure 5: Phase diagram at the unitarity point for equal masses as obtained from the virial expansion to second order: (thin line) and (thick). The gas is mixed above the lines, and phase separated below.
Comments 0
Request Comment
You are adding the first comment!
How to quickly get a good reply:
  • Give credit where it’s due by listing out the positive aspects of a paper before getting into which changes should be made.
  • Be specific in your critique, and provide supporting evidence with appropriate references to substantiate general statements.
  • Your comment should inspire ideas to flow and help the author improves the paper.

The better we are at sharing our knowledge with each other, the faster we move forward.
The feedback must be of minimum 40 characters and the title a minimum of 5 characters
Add comment
Loading ...
This is a comment super asjknd jkasnjk adsnkj
The feedback must be of minumum 40 characters
The feedback must be of minumum 40 characters

You are asking your first question!
How to quickly get a good answer:
  • Keep your question short and to the point
  • Check for grammar or spelling errors.
  • Phrase it like a question
Test description