Spin ice under pressure: symmetry enhancement and infinite order multicriticality

Spin ice under pressure: symmetry enhancement and infinite order multicriticality

L. D. C. Jaubert, J. T. Chalker, P. C. W. Holdsworth, and R. Moessner Max-Planck-Institut für Physik komplexer Systeme, 01187 Dresden, Germany. Theoretical Physics, Oxford University, 1 Keble Road, Oxford, OX1 3NP, United Kingdom. Laboratoire de Physique, École Normale Supérieure de Lyon, Université de Lyon, CNRS, 46 Allée d’Italie, 69364 Lyon Cedex 07, France.
July 26, 2019
Abstract

We study the low-temperature behaviour of spin ice when uniaxial pressure induces a tetragonal distortion. There is a phase transition between a Coulomb liquid and a fully magnetised phase. Unusually, it combines features of discontinuous and continuous transitions: the order parameter exhibits a jump, but this is accompanied by a divergent susceptibility and vanishing domain wall tension. All these aspects can be understood as a consequence of an emergent SU(2) symmetry at the critical point. We map out a possible experimental realisation.

pacs:
05.50.+q 05.70.Jk 75.10.Hk 75.40.Cx 75.40.Mg

One fascinating aspect of condensed matter physics is the extent to which the nature and symmetries of emergent low-energy degrees of freedom can be independent of the high energy ones from which they derive. While many types of low energy degrees of freedom are possible, systems in which these correspond to a gauge field are still rare.

In this paper we study this theme in a setting which brings forth an unusual sequence of low energy fluctuations and symmetries: we consider spin ice, a frustrated Ising magnet on the pyrochlore lattice, whose low temperature behaviour is well-described by a gauge field, an emergent magnetostatics, representing a so-called Coulomb phase where correlations decay algebraically as . Transitions out of such a phase have attracted a great deal of attention recently Henley09 (); Alet06a (); Pickles08a (); Chen09 ().

We ask what happens when the host crystal is subjected to uniaxial pressure. This is a powerful probe of correlated matter, which has previously produced interesting information in frustrated magnets closely related to spin ice Mirebeau02a (); Mirebeau06a (). Specifically, we consider the case of pressure-induced strain that lowers the crystal symmetry from cubic to tetragonal. We find that this induces a highly unusual symmetry-breaking phase transition out of the Coulomb phase: it is characterised by discontinuities in quantities such as the magnetisation, without being first order. Rather, it occurs at an infinite order multicritical point and is accompanied by a divergent susceptibility. We demonstrate both these features using Monte Carlo simulations. Further salient properties of the critical point include the absence of a domain wall tension, along with spin correlations that vanish in a plane perpendicular to the strain-induced tetragonal axis. These should be observable experimentally, and we discuss the scope for realising such a transition in the laboratory.

The unusual nature of the transition is a consequence of an emergent SU(2) symmetry: as the pressure reduces the symmetry of the external space, an enhanced internal symmetry appears. We show this by means of an exact solution in three dimensions at the critical temperature and a mapping to a quantum phase transition in dimensions, between Ising and XY anisotropy in a spin- ferromagnet.

Transitions with analogous features have been studied previously in the context of ferroelectrics LinesGlass (), using versions of the model for potassium dihydrogen phosphate (KDP) introduced by Slater Slater41 (), which in its two dimensional form is equivalent to the 6-vertex model and exactly solved Lieb67d (). Spin ice has the potential to provide a much cleaner realisation of this physics than the transition in ferroelectrics, since its magnetic degrees of freedom are much more accurately represented by Ising variables supported on a rigid lattice.

Spin ice is well modelled by Ising spins parallel to their local easy-axis on the pyrochlore lattice Harris97a (). At sufficiently low temperature we can limit ourselves to the highly degenerate ground state ensemble with two spins pointing in and two out of each tetrahedron (ice-rules) and consider effective nearest neighbour interactions Gingras01a (); Isakov05a (). After coarse-graining the magnetisation, the discrete ice-rules can be written in terms of a continuous divergence free condition from which emerge the algebraic correlations Isakov04b (); Henley05a (). Our goal is to lift the degeneracy of the resulting Coulomb phase via the exchange modulation

(1)

where for bonds on planes perpendicular to the strain axis, and otherwise (see Fig. 1). For , the symmetry of this Hamiltonian is spontaneously broken at temperature in favour of a state magnetised parallel to the [001] direction. If the strain were very large, so that , ordering would be from a conventional paramagnetic state and in the standard three-dimensional Ising universality class. In contrast, for realistic, small strains is much less than and ordering is from the Coulomb phase, with the striking features we describe.

Figure 1: A tetrahedron of the pyrochlore lattice with exchange and as indicated: the dashed bonds lie in (001) planes. One of the two ground states for is shown.

We first present results from Monte Carlo simulations, done with a worm algorithmIsakov04a (); Jaubert09c () in which loop updates preserve the divergence free nature of the magnetisation. The temperature dependence of the magnetisation and of the inverse susceptibility are shown in Fig. 2, upper panel: remarkably, takes its saturation value at all temperatures below , but diverges as is approached from above. To better characterise the transition, we also examine the probability distribution function (PDF) of the order parameter, shown in Fig. 2, lower panel. This is a standard diagnostic: two peaks are expected in the PDF at the transition point when this is first order, but only one peak if it is continuous Binder87 (). Again, we find unconventional behaviour: a PDF that is uniform over all values of at .

An exactly uniform order parameter distribution arises within Landau theory as a limiting case. The free energy density close to a multicritical point of order is

(2)

In the limit , it is independent of at . Moreover, the order parameter exponent takes the value , generating a jump for . Also, the susceptibility ( for ) has an exponent independent of and an amplitude ratio that vanishes as . All these are borne out by our simulations. This success of mean field theory reflects the exceptional value of the upper critical dimension, , which follows from standard arguments with allowance for the anisotropic spatial scaling, see Eq 5 below.

In previous discussions of the ferroelectric KDP model LinesGlass (); Slater41 (); Takahashi41 (); Takagi48b (); Nagle69a (); Shore94a () some distinctive aspects have been recognised. Indeed, Slater’s original approximation Slater41 () yields a free energy independent of the order parameter at the transition, which on this basis has been called infinite order Benguigui77a (). Such a conclusion is evidently very delicate Takahashi41 (), and corrections to the approximation or physical perturbations have the potential to convert the transition into a conventional one: either first order or continuous. This is in fact the case for the material KDP itself, which has a first order transition that can be driven through a tricritical point under pressure LinesGlass (). While in two dimensions, an exact solution of the KDP model corroborates the main features of Slater’s results Lieb67d (); Shore94a (); Baxter07a (), it is not a priori clear – not least in view of the famous difficulties in generalising Onsager’s solution of the Ising model – what this tells us for higher dimension. Here we present simulations and exact results for the transition in three dimensions. In addition, we show how to realise it in a magnetic material.

Figure 2: (Color online) Top: Simulation data for (blue circles) and (red triangles) vs. . Bottom: PDF of at different temperatures. For (red) the PDF has two sharp peaks at . For (black) the PDF is broad in small samples (dashed black line for ) and almost flat in larger samples (solid black line for and ). For (blue) the PDF is Gaussian. (Values at scaled to fit on vertical axis.)

The ice rules impose the same value of the magnetisation in all planes: any configuration can be mapped onto an ensemble of strings of down spins spanning the system from top to bottom, with the convention that the string vacuum is the state in which all spins are up Takahashi41 (). The number of strings defines the total magnetisation and a topological sector, so that the former can be used to label the latter. The equiprobability of all sectors (see Fig. 2) already suggests the absence of interactions between strings. This observation can be made precise using the transfer matrix that acts between two adjacent (001) layers of the lattice Powell08a (). Since this transfer matrix is a direct product of factors representing separate tetrahedra, we first discuss a single tetrahedron. A single string can enter the tetrahedron at either site in one layer and leave it at either site in the other layer, with energy cost . This sector is therefore represented in by a block in which all entries are the Boltzmann factor . By contrast, zero or two strings in a tetrahedron cost no energy and impose the next configuration locally, generating two blocks with unit entries in , which hence has the form

(3)

The maximum eigenvalues of lie for in the two fully magnetised sectors, but for all sectors have the same maximal eigenvalue. In addition, the associated eigenvector in the one-string sector is . Explicit calculation of the transfer matrix for a complete lattice is complicated by the fact that the repeat unit in the direction involves four different layers. Nevertheless, its maximal eigenvalues inherit precisely the properties described for , and at the associated eigenvectors in each sector give equal weight to all arrangements of strings on a layer. The maximal eigenvalues determine the physical properties for a system of size if the dimension satisfies . As a result: (i) below the magnetisation is saturated; and (ii) at all sectors are equiprobable and all configurations within a sector are equiprobable, reflecting the absence of interactions between strings Jaubert09c (). By contrast, for a system with subleading eigenvalues also contribute and the PDF for is rounded, as is apparent in Fig. 2.

The transfer matrix for the complete lattice can alternatively be thought of as the evolution operator in imaginary time for a two-dimensional quantum model (in analogy with Eq. (8) of Lieb67d ()) with Hamiltonian

(4)

The strings thus denote the world lines of spins. In this language the decomposition into sectors is a consequence of the conservation of total , and is due to a U(1) symmetry. The ground state of has ferromagnetic order of the quantum spins for all , with an orientation for the magnetisation that depends on . For , spins lie in the - plane and the state has zero-point fluctuations, representing the Coulomb phase. For , spins are aligned along the -axis and the state has no fluctuations, representing the low temperature phase of the classical system. The equiprobability of string sectors at the critical point corresponds here to the degeneracy of the ground states of the isotropic Heisenberg ferromagnet with spins, for all values of the total magnetisation . We have confirmed that this isotropy is a property of the full transfer matrix, and not only of the leading eigenvectors, by checking that the matrix commutes with the total spin raising and lowering operators, . This constitutes an enhancement of the symmetry at the critical point from U(1) to SU(2).

The quantum description can be employed to calculate correlation functions within a given sector in spin ice, by approximating the imaginary time direction as continuous and treating using harmonic spinwave theory. For a system of shape sufficiently anisotropic () to justify a ground state treatment of the 2+1 dimensional problem, and taking and to denote distances along the [001] direction and in the (001) plane respectively, with a microscopic length, two-point correlations at are

(5)

As the strings do not interact, this form reflects the string auto-correlations present in a random walk in two dimensions with propagation time . It agrees well with results from simulations, as we show in Fig. 3.

Figure 3: (Color online) Main panel: Behaviour of vs , on a semi-log scale for (), 2 (), 4 (), 6 (), 8 (), 10 (). Dashed line shows behaviour expected from Eq. (5). The system size is and . Inset: Same data plotted as vs on a linear scale, showing that correlations vanish within (001) planes.

A further consequence of the absence of interactions between strings is that the surface tension between oppositely magnetised domains vanishes and the domain wall width diverges, as is approached from below. We investigate this phenomenon in simulations by using weak, position-dependent magnetic fields to induce two domains with the interfaces between them lying on average in the - plane. Results are shown in Fig. 4. At the magnetisation profile is a function only of . Below a mean field treatment of gives a domain wall width : this is confirmed in Fig. 4, up to a constant vanishing in the thermodynamic limit. It is striking to find broad domain walls in an Ising magnet; they may be detectable using small angle neutron scattering.

Figure 4: Left: Magnetisation profile vs at for . Right: Domain wall width vs for . The straight line is a guide to the eye. All samples have .

The natural way to generate the required degeneracy lifting in a magnetic compound is to apply uniaxial pressure along the [001] axis of a single crystal. We require positive. Within the nearest neighbour approximation the effective coupling has two contributions, one from the long-range dipolar interactions Siddharthan99a (); Gingras01a (); Isakov05a (), the other due to superexchange. While a uniaxial compression along [001] increases the former, the change of the latter is less clear as it depends on the evolution of orbital overlaps.

Figure 5: Percentage change in magnetisation measured under uniaxial pressure of kbar, , compared to that at atmospheric pressure, , at K as a function of applied field along the axis (extracted from Mito07a ()).

Results from the one experiment so far performed on DyTiO under pressure Mito07a () suggest that the effective coupling is indeed modified so as to produce . Pressure causes a increase in at small field, but a decrease at high field (Fig. 5). The increase in the zero field susceptibility is consistent with the lifting of the degeneracy in favour of the states with magnetization along the field axis, as required for the transition studied here (Fig. 1). The reduction of the saturated moment is expected as the crystal is squeezed along [001] because of a resulting tilt of the easy axes away from [001].

In fitting the parameter , we account for demagnetisation effects by modelling the sample as a prolate ellipsoid with major axes given by the dimensions of the approximately rectangular parallelepiped specimen. For the interaction parameter of DyTiO Hertog00a (), the best fit, shown in Fig. 5, yields mK.

Whereas this temperature is comfortably within reach of cryogenics, the dynamics of spin ice slows down greatly below mK, as activated ice-rule violating defects disappear. Their presence thus appears indispensable in practice, even though they will lead to more standard second-order phase transition in the three dimensional Ising universality class Takagi48b (); Jaubert09c (). The width of its critical region will, however, vanish with defect concentration. Experiments should thus aim at the lowest dynamically accessible transition temperatures, with the target mK only a factor of 3 away from existing experiments Mito07a (). We hope our work will stimulate further experimental efforts to realise this unusual transition.

We thank K. Matsuhira for sharing results from Ref. Mito07a (), and D. Simon and S.T. Bramwell for useful discussions. We acknowledge financial support from ESF under Grant PESC/RNP/HFM (PCWH and LJ), from ANR under Grant 05-BLAN-0105 (LJ), and from EPSRC (JTC) under Grant EP/D050952/1.

References

  • (1) C. L. Henley, arXiv:0912.4531 (2009).
  • (2) F. Alet et al., Phys. Rev. Lett. 97, 030403 (2006).
  • (3) T. S. Pickles, T. E. Saunders, and J. T. Chalker, Europhys. Lett. 84, 36002 (2008).
  • (4) G. Chen et al., Phys. Rev. B 80, 045112 (2009).
  • (5) I. Mirebeau et al., Nature 420, 54 (2002).
  • (6) I. Mirebeau et al., Phys. Rev. B 74, 174414 (2006).
  • (7) M. E. Lines and A. M. Glass, Principles and Applications of Ferroelectrics and Related Materials (Clarendon, Oxford, 1977).
  • (8) J. C. Slater, J. Chem. Phys. 9, 16 (1941).
  • (9) E. H. Lieb, Phys. Rev. Lett. 19, 108 (1967).
  • (10) M. J. Harris et al., Phys. Rev. Lett. 79, 2554 (1997).
  • (11) M. J. P. Gingras and B. C. den Hertog, Can. J. Phys. 79, 1339 (2001).
  • (12) S. V. Isakov, R. Moessner and S. L. Sondhi, Phys. Rev. Lett. 95, 217201 (2005).
  • (13) S. V. Isakov et al., Phys. Rev. Lett. 93, 167204 (2004).
  • (14) C. L. Henley, Phys. Rev. B 71, 014424 (2005).
  • (15) S. V. Isakov et al., Phys. Rev. B 70, 104418 (2004).
  • (16) L. D. C. Jaubert , Ph.D. thesis, ENS de Lyon (2009).
  • (17) K. Binder, Rep. Prog. Phys. 50, 783 (1987).
  • (18) H. Takahashi, Proc. Phys. Math. Soc. Japan 23, 1096 (1941).
  • (19) Y. Takagi, J. Phys. Soc. Jpn 3, 273 (1948).
  • (20) J. F. Nagle, Comm. Math. Phys. 13, 62 (1969).
  • (21) J. D. Shore and D. J. Bukman, Phys. Rev. Lett. 72, 604 (1994).
  • (22) L. Benguigui, Phys. Rev. B 16, 1266 (1977).
  • (23) R. J. Baxter, Exactly Solved Models in Statistical Mechanics (Dover Publications, Mineola, 2007), Chap. 8.
  • (24) S. Powell and J. T. Chalker, Phys. Rev. B 78, 024422 (2008).
  • (25) R. Siddharthan et al., Phys. Rev. Lett. 83, 1854 (1999).
  • (26) M. Mito et al., J. Magn. Magn. Mater. 310, E432 (2007).
  • (27) B. C. den Hertog and M. J. P. Gingras, Phys. Rev. Lett. 84, 3430 (2000).
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
Cancel
Loading ...
267941
This is a comment super asjknd jkasnjk adsnkj
Upvote
Downvote
""
The feedback must be of minumum 40 characters
The feedback must be of minumum 40 characters
Submit
Cancel

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
Test description