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REVIEW 2 major objections 5 minor 36 references

Emergent Snake Magnetic Domains in Canted Kagome Ice

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Pith's one-line read A field quench can trap canted kagome ice in long-lived snake domains whose edge spins make localized monopole–antimonopole pairs.

desk verdict A new d-vortex ground state and snake-domain metastability with a real kinetic claim that currently lacks the barrier calculation or scaling evidence to make it stick in the thermodynamic limit. read the letter →

arxiv 1908.05872 v1 pith:VUCZTK6C submitted 2019-08-16 cond-mat.stat-mech cond-mat.str-el

Wen-Han Kao , Gia-Wei Chern , Ying-Jer Kao This is my paper · ORCID
classification cond-mat.stat-mechcond-mat.str-el MSC 82B2082C80 PACS 75.10.Hk75.40.Mg
keywords kagomeicespinsnakedomainsmagneticmonopolesmetastabilitykineticMonteCarlogeometricalfrustrationfieldquench
verification ladder T0 review T1 audit T2 compute T3 formal

The pith

A machine-rendered reading of the paper's core claim, the machinery that carries it, and where it could break.

The reading

This paper argues that in a two-dimensional kagome-ice magnet with canted moments and competing further-neighbor interactions, a magnetic-field quench from the saturated state can leave the system stuck in long-lived 'snake' domains instead of reaching the stripe ground state. The snake is a metastable mixed-phase texture living at the boundary between vortex and stripe order; its interior spins are frozen, while spins on its edges flip easily and create and annihilate localized monopole–antimonopole pairs. Because a broken snake can only grow or shrink by moving single monopoles along its endpoints, the excitations are both confined and effectively immobile, and the system relaxes only extremely slowly. If this is right, it explains the smeared, diffuse neutron scattering observed in tilted-field spin ice without long-range stripe order, and it suggests that field history can be used to manipulate spin and charge textures in artificial kagome arrays.

What carries the argument

The load-bearing object is the snake domain: a winding string excitation on the stripe background decorated by a series of non-winding hexagon-loop excitations, so it costs less energy than a bare string and can take any odd width $w \ge 3$. A snake has a chirality, and the ice rule forces the kink spins on its edges to point against the in-plane field; flipping one edge spin costs $\Delta E_e = 8J_1 + 4J_2 + 4J_{3a} + 4J_{3b} - \frac{2}{3}h_\perp - \frac{2\sqrt{2}}{3}h_\parallel$ and creates a localized triple-charge pair. The total energy of $n$ snakes and $m$ edge excitations is $E_{n,m} = E_{\mathrm{stripe}} + n\Delta E_s L + m\Delta E_e$, whose special cases $n = L/3, m=0$ recover the vortex state and $n = L/3, m = nL$ recover the defected-vortex state. The kinetic bottleneck is the mechanism that makes the metastability work: a broken snake can only relax by migrating a monopole along its endpoint, and the waiting-time Monte Carlo dynamics used in the study contains no cooperative loop move that bypasses this barrier.

What would settle it

Run the same field quench with a Monte Carlo update that includes cooperative loop flips as well as single-spin flips; if snake domains then relax to the uniform stripe state on a short timescale at $L \sim 72$, the long-lived metastability would be an artifact of the single-spin-flip update rather than a physical energy barrier. An experimental counterpart is a time-resolved neutron-scattering quench on a tilted-field kagome system: the diffuse peak intensity should migrate toward the stripe Bragg position on an accessible timescale if the snakes are not truly stuck.

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Extended reading notes

Core claim

On the paper's own terms, the central discovery is that the coexistence regime between the vortex and stripe phases contains winding snake domains that are lower in energy than the elementary string excitation because each snake is a string dressed by non-winding hexagon loops. These snakes have odd widths at least three, are degenerate in width, and cost $\Delta E_s = 12J_2 - 12J_{3a} - 2\sqrt{2}h_\parallel$ per unit length relative to the stripe state, so a perfect snake costs energy proportional to the lattice size and is not the equilibrium ground state. Metastability is kinetic: in single-spin-flip dynamics a snake can only grow or shrink by migration of a single monopole at its endpoint, and although the edge kink spins are easily flipped, the resulting triple-charge (monopole–antimonopole) pairs cannot propagate into the snake interior. The paper characterizes the trapped state as a mixture of the vortex, stripe, and defected-vortex states, reconstructs the snake number and edge-excitation number from simple order parameters, and shows that the magnetic structure factor peaks between the vortex-corner and stripe-edge-center Bragg positions, a fingerprint of a frozen topological sector. It connects this pattern to the diffuse scattering observed in tilted-field pyrochlore spin ice.

Load-bearing premise

The argument rests on the kinetic assumption that a snake can only grow or shrink by migration of single magnetic charges (monopoles) at its endpoints, with no cooperative loop or multi-spin relaxation channel available; if such a channel exists, the snake's energy cost, which grows with system size, would let it decay.

Editorial extensions

If this is right

  • Field-quenched samples near the vortex-stripe boundary can remain in mixed snake textures for times far beyond ordinary Monte Carlo runs, so the final configuration depends on the quench history and not just on temperature and field.
  • The magnetic structure factor of the snake phase shows horizontally smeared diffuse scattering with peak intensity between the vortex-corner and stripe-edge-center Bragg positions, giving a concrete neutron-scattering fingerprint.
  • Edge thermal fluctuations generate localized monopole–antimonopole pairs whose number grows monotonically with temperature, while the snake density is controlled by the third-neighbor coupling $J_{3a}$, so the two can be tuned independently.
  • The mixed snake state is a coexistence of the vortex, stripe, and defected-vortex ground states, so the first-order vortex-stripe transition proceeds through elongated anisotropic domains rather than isotropic nuclei.
  • In artificial kagome ice, where domains and triple charges can be imaged directly, the snake texture offers a route to manipulating both spin and charge patterns through field history.

Reading between the lines

Editorial extensions of the paper, not claims the author makes directly.

  • If the single-monopole bottleneck is the true relaxation mechanism, then the anisotropic shape of snakes implies the vortex-stripe transition has strongly direction-dependent nucleation rates; measurements of domain-size anisotropy after quenches would test this directly.
  • A natural testable extension is to add a cooperative loop update to the Monte Carlo: if snakes then anneal quickly to the stripe state, the long lifetimes are an artifact of single-spin-flip kinetics rather than a robust physical energy barrier.
  • The same mechanism, a winding defect dressed by non-winding loop excitations, could be generic to frustrated Ising models with competing further-neighbor couplings, suggesting snake-like metastable textures may appear in other kagome-derived magnets beyond this parameter set.
  • Artificial spin-ice arrays with tunable effective third-neighbor couplings might be engineered to set the snake density and edge-excitation rate, turning the metastable texture into a controllable source of localized magnetic charges.
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Editorial analysis

A structured set of objections, weighed in public.

Desk editor's note, referee report, and a circularity audit.

Referee Report

2 major / 5 minor

Summary. The paper studies a two-dimensional kagome-ice model with Ising moments canted along pyrochlore local (111) axes, including second- and third-neighbor exchange and both out-of-plane and in-plane fields. Using equilibrium Monte Carlo, the authors map out low-temperature phases—vortex, stripe, and a newly identified defected-vortex state—and locate the phase boundaries. They then use a rejection-free waiting-time Monte Carlo method to simulate field quenches from the saturated state and observe a five-stage relaxation, with many runs becoming trapped in long-lived 'snake' domains. The paper characterizes these domains energetically, showing that snake energy grows linearly with system size, and proposes that edge spins fluctuate locally, creating localized monopole-antimonopole pairs that cannot propagate. The authors compare the computed structure factor with neutron scattering in tilted-field spin ice and discuss implications for artificial kagome ice.

Significance. If the metastability claim survives scrutiny, the paper is a useful contribution: it identifies a disorder-free mechanism for extremely slow relaxation in a frustrated spin model, provides explicit energetic formulas for snake and edge excitations, and connects the resulting diffuse scattering to a known experimental puzzle. The simulations are self-contained, with no parameter fitting to experimental data, and the waiting-time Monte Carlo method is a suitable tool for the timescale problem. The main limitation is that the central kinetic bottleneck is asserted rather than demonstrated; the thermodynamic-limit and quantitative claims therefore need additional support.

major comments (2)
  1. [Section V, Eq. (10)] The central claim of extremely long-lived snake domains rests on a kinetic bottleneck that is asserted but not quantified. Equation (10) makes all odd-width snakes degenerate, so a snake boundary can be displaced laterally at zero energy cost; a coherent shift by one step requires an intermediate energy proportional to L under single-spin-flip dynamics, but the paper does not rule out other cooperative or multi-spin relaxation channels. The text states that a broken snake can only migrate by single-monopole hops at its endpoints and that edge triple charges can hardly diffuse, yet no activation energies for these moves are computed; Eq. (11) gives only the cost of flipping one edge spin from the ground state, not the barrier to move a charge along the edge or to move an endpoint. Since the thermodynamic-limit stability of the snakes depends on this bottleneck, I request either explicit saddle-point barrier calculations for the relevant moves (including a lateral snake shift) or system-size scaling of the escape rate from the trapped state.
  2. [Section IV, Figs. 3 and 5(f)] The numerical evidence for 'extremely long relaxation time' is based on a single lattice size (L=72), a single parameter set, 10^5 waiting-time steps, and 100 samples, with no error bars reported in Figs. 3 and 5(f). These statistics cannot distinguish a genuine kinetic trap from slow finite-size relaxation, especially because Eq. (10) makes the energy of a perfect snake grow with L; the text claims the bottleneck persists 'even in larger system sizes' without showing any L dependence. Please add finite-size scaling of the trapped fraction and of the time-dependent order parameters, and error estimates for the reported densities.
minor comments (5)
  1. [Figs. 3 and 5(f)] The figures would be easier to interpret with error bars or with a statement that the statistical error is smaller than the symbol size.
  2. [Fig. 4 caption] The caption distinguishes runs that 'can reach the stripe state' from those 'getting stuck'; please specify the quantitative criterion used to classify a run into either group.
  3. [Section V, Eq. (13)] Equation (13) is presented without derivation; a short explanation of how n and m follow from Q_t and O_k would help readers.
  4. [Fig. 2 caption] The 'shaded region' where snake metastable states occur is not visible in the printed figure; please mark the relevant parameter region explicitly.
  5. [Section II] The third-neighbor couplings J3a and J3b are not defined geometrically; a sentence or diagram specifying the two types of third-neighbor paths would improve reproducibility.

Circularity Check

0 steps flagged · score 1.0 of 10

No material circularity: the energetic and Monte Carlo analysis is self-contained, and the few self-citations are background only.

full rationale

The central derivation chain is self-contained. The Hamiltonian and charge variables define the model; the phase boundaries are calculated directly from energy differences of the Hamiltonian (h_perp,c = 12J1 + 12J3a + 6J3b; h_parallel,c = 3*sqrt(2)J2 - 3*sqrt(2)J3a), and the equilibrium Monte Carlo results independently evaluate those phases. The snake energy formula (Eq. 10), edge-excitation energy (Eq. 11), and mixed-state energy (Eq. 12) are explicit energetic decompositions of stated configurations rather than fitted parameters, and Eq. (13) merely re-expresses the measured charge and kink order parameters as snake/edge-excitation counts. No experimental data are used to tune the model; the neutron-scattering comparison is qualitative and not used as an input. The cited [25] is by two of the present authors but is used only as background for the q=X interpretation, and [27,28] are used only to identify known vortex-state physics; neither carries the metastability argument. The endpoint-only kinetic bottleneck invoked around Eq. (10) is an unverified physical assumption and therefore a correctness risk, but it is not circular: the simulations do not fit that bottleneck into the model, and no prediction is equivalent by construction to an input.

Assumptions & free parameters 5 free parameters · 4 assumptions · 0 invented entities

The model has no free parameters fitted to data; all coupling constants and fields are hand-selected inputs defining the model. The key assumption is that the single-spin-flip kinetic Monte Carlo dynamics with these parameters captures the physical relaxation mechanism; if loop or multi-spin processes were active, the snake domains might equilibrate on accessible timescales. No new fundamental entities are introduced.

free parameters (5)
  • J2 = -1/3
    Second-neighbor exchange coupling fixed by hand to place the system near the stripe-vortex competition; all phase diagrams use J2=-1/3.
  • J3a = 0.05 (main kinetic study); varied in Fig. 2(b)
    Third-neighbor coupling chosen near the vortex-stripe boundary; WTM simulation uses J3a=0.05.
  • J3b = 0 (main kinetic study); varied in Fig. 2(b)
    Third-neighbor coupling b set to 0 for the main kinetic study.
  • h_perp = 11.76
    Out-of-plane field chosen just below the saturation field (h_perp,c ~ 11.96 for the chosen parameters) to favor the stripe state after the quench.
  • h_parallel = -1.68
    In-plane field chosen slightly below h_parallel,c ~ -1.41 to land near the stripe-vortex boundary; negative denotes tilt toward [11-2].
assumptions (4)
  • domain assumption Classical Ising spins rigidly aligned to local <111> easy axes describe the physics (Hamiltonian Eq. 1).
    The entire model is classical Ising; quantum fluctuations are ignored, which is standard for pyrochlore spin-ice modeling.
  • domain assumption The kagome ice rule is the relevant low-energy constraint except for the deliberately constructed d-vortex defects.
    Section III defines charges Q and describes ground states as satisfying the ice rule, with the d-vortex state containing one-third triple-charge defects.
  • ad hoc to paper Single-spin-flip waiting-time Monte Carlo with Boltzmann weights captures the physical field-quench dynamics; cooperative or loop moves are negligible.
    Section IV uses the waiting-time method and explicitly notes that loop algorithms cannot handle the metastability; the absence of multi-spin relaxation channels is a modeling assumption.
  • ad hoc to paper The chosen couplings (J2=-1/3, J3a≈0.05, h_perp=11.76, h_parallel=-1.68) place the system near a first-order boundary in a regime representative of real spin-ice materials.
    These parameters are hand-selected to sit near the vortex-stripe boundary; the experimental relevance claim depends on this regime being physically accessible.

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Cite this review

Pith. "Pith review of Emergent Snake Magnetic Domains in Canted Kagome Ice." pith.science (2026). https://pith.science/paper/VUCZTK6C

@misc{pith2026190805872,
  author       = {Pith},
  title        = {Pith review of: Emergent Snake Magnetic Domains in Canted Kagome Ice},
  year         = {2026},
  howpublished = {\url{https://pith.science/paper/VUCZTK6C}},
  note         = {Machine review of arXiv:1908.05872}
}
abstract

We study the two-dimensional kagome-ice model derived from a pyrochlore lattice with second- and third-neighbor interactions. The canted moments align along the local $\langle 111 \rangle$ axes of the pyrochlore and respond to both in-plane and out-of-plane external fields. We find that the combination of further-neighbor interactions together with the external fields introduces a rich phase diagram with different spin textures. Close to the phase boundaries, metastable $\textit{"snake"}$ domains emerge with extremely long relaxation time. Our kinetic Monte Carlo analysis of the magnetic-field quench process from saturated state shows unusually slow dynamics. Despite that the interior spins are almost frozen in snake domains, the spins on the edge are free to fluctuate locally, leading to frequent creation and annihilation of monopole-anti-monopole bound states. Once the domains are formed, these excitations are localized and can hardly propagate due to the energy barrier of snakes. The emergence of such snake domains may shed light on the experimental observation of dipolar spin ice under tilted fields, and provide a new strategy to manipulate both spin and charge textures in artificial spin ice.

Figures

Figures reproduced from arXiv: 1908.05872 by the authors.

Figure 1
Figure 1. FIG. 1. Canted kagome ice model. (a) The easy direction of each [PITH_FULL_IMAGE:figures/full_fig_p002_1.png] view at source ↗
Figure 2
Figure 2. FIG. 2. Energetic phase diagrams and corresponding ground-state [PITH_FULL_IMAGE:figures/full_fig_p003_2.png] view at source ↗
Figure 3
Figure 3. FIG. 3. Equilibrium Monte Carlo results. (a) Charge density and (b) vortex-state order parameter of [PITH_FULL_IMAGE:figures/full_fig_p004_3.png] view at source ↗
Figures from the paper (3 more)
Figure 4
Figure 4. Figure 4: FIG. 4. Field-quench process from the saturated state by wait [PITH_FULL_IMAGE:figures/full_fig_p005_4.png]
Figure 5
Figure 5. Figure 5: FIG. 5. (a) Single string excitation on the background of the stripe state. (b) Single snake of width = 3. (c) Single snake of width = 5. (d) [PITH_FULL_IMAGE:figures/full_fig_p006_5.png]
Figure 6
Figure 6. Figure 6: FIG. 6. Magnetic structure factor of the (a) vortex state (b) stripe state and (c) snake phase. Note that in (c), the highest-intensity points on the [PITH_FULL_IMAGE:figures/full_fig_p008_6.png]

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Works this paper leans on

36 extracted references · 33 canonical work pages

  1. [25]

    W.-H. Kao, P. C. W. Holdsworth, and Y .-J. Kao, Phys. Rev. B 93, 180410 (2016)

    work page 2016

  2. [1]

    S. F. Edwards and P. W. Anderson, J. Phys. F: Met. Phys.5, 965 (1975)

    work page 1975

  3. [2]

    M. J. Harris, S. T. Bramwell, D. F. McMorrow, T. Zeiske, and K. W. Godfrey, Phys. Rev. Lett.79, 2554 (1997). 8 FIG. 6. Magnetic structure factor of the (a) vortex state (b) stripe state and (c) snake phase. Note that in (c), the highest-intensity points on the edge of Brillouin zone locate at somewhere between the corner and edge-center, which are the pos...

    work page 1997

  4. [3]

    A. P. Ramirez, A. Hayashi, R. J. Cava, R. Siddharthan, and B. S. Shastry, Nature 399, 333 (1999)

    1999

  5. [4]

    S. V . Isakov, K. Gregor, R. Moessner, and S. L. Sondhi, Phys. Rev. Lett. 93, 167204 (2004)

    2004

  6. [5]

    S. V . Isakov, R. Moessner, and S. L. Sondhi, Phys. Rev. Lett. 95, 217201 (2005)

    work page 2005

  7. [6]

    R. G. Melko, B. C. den Hertog, and M. J. P. Gingras, Phys. Rev. Lett. 87, 067203 (2001)

    work page 2001

  8. [7]

    Castelnovo, R

    C. Castelnovo, R. Moessner, and S. L. Sondhi, Nature 451, 42 (2008)

    2008

Show all 36 references
  1. [8]

    D. J. P. Morris, D. A. Tennant, S. A. Grigera, B. Klemke, C. Castelnovo, R. Moessner, C. Czternasty, M. Meissner, K. C. Rule, J.-U. Hoffmann, K. Kiefer, S. Gerischer, D. Slobinsky, and R. S. Perry, Science 326, 411 (2009)

    2009

  2. [9]

    C. L. Henley, Annu. Rev. Condens. Matter Phys 1, 179 (2010)

    2010

  3. [10]

    Fennell, P

    T. Fennell, P. P. Deen, A. R. Wildes, K. Schmalzl, D. Prab- hakaran, A. T. Boothroyd, R. J. Aldus, D. F. McMorrow, and S. T. Bramwell, Science 326, 415 (2009)

    2009

  4. [11]

    Brooks-Bartlett, S

    M. Brooks-Bartlett, S. T. Banks, L. D. Jaubert, A. Harman- Clarke, and P. C. Holdsworth, Phys. Rev. X 4, 011007 (2014)

    2014

  5. [12]

    Petit, E

    S. Petit, E. Lhotel, B. Canals, M. Ciomaga Hatnean, J. Ollivier, H. Mutka, E. Ressouche, A. R. Wildes, M. R. Lees, and G. Bal- akrishnan, Nat. Phys. 12, 746 (2016)

    2016

  6. [13]

    Z. L. Dun, J. Trinh, K. Li, M. Lee, K. W. Chen, R. Baumbach, Y . F. Hu, Y . X. Wang, E. S. Choi, B. S. Shastry, A. P. Ramirez, and H. D. Zhou, Phys. Rev. Lett. 116, 157201 (2016)

    2016

  7. [14]

    J. A. Paddison, H. S. Ong, J. O. Hamp, P. Mukherjee, X. Bai, M. G. Tucker, N. P. Butch, C. Castelnovo, M. Mourigal, and S. E. Dutton, Nat. Commun. 7, 13842 (2016)

    2016

  8. [15]

    Canals, I.-A

    B. Canals, I.-A. Chioar, V .-D. Nguyen, M. Hehn, D. Lacour, F. Montaigne, A. Locatelli, T. O. Mentes ¸, B. S. Burgos, and N. Rougemaille, Nat. Commun. 7, 11446 (2016)

    2016

  9. [16]

    Udagawa, L

    M. Udagawa, L. Jaubert, C. Castelnovo, and R. Moessner, Phys. Rev. B 94, 104416 (2016)

    2016

  10. [17]

    Mizoguchi, L

    T. Mizoguchi, L. D. Jaubert, and M. Udagawa, Phys. Rev. Lett. 119, 077207 (2017)

    2017

  11. [18]

    Chioar, N

    I. Chioar, N. Rougemaille, and B. Canals, Phys. Rev. B 93, 214410 (2016)

    2016

  12. [19]

    Smerald, S

    A. Smerald, S. Korshunov, and F. Mila, Phys. Rev. Lett. 116, 197201 (2016)

    2016

  13. [20]

    Mellado, O

    P. Mellado, O. Petrova, Y . Shen, and O. Tchernyshyov, Phys. Rev. Lett. 105, 187206 (2010)

    2010

  14. [21]

    Chioar, B

    I. Chioar, B. Canals, D. Lacour, M. Hehn, B. S. Burgos, T. Mentes ¸, A. Locatelli, F. Montaigne, and N. Rougemaille, Phys. Rev. B 90, 220407 (2014)

    2014

  15. [22]

    Montaigne, D

    F. Montaigne, D. Lacour, I. A. Chioar, N. Rougemaille, D. Louis, S. M. Murtry, H. Riahi, B. S. Burgos, T. O. Mentes ¸, A. Locatelli, B. Canals, and M. Hehn, Sci. Rep.4, 5702 (2014)

    2014

  16. [23]

    Matsuhira, Z

    K. Matsuhira, Z. Hiroi, T. Tayama, S. Takagi, and T. Sakak- ibara, J. Phys.: Condens. Matter 14, L559 (2002)

    2002

  17. [24]

    Fennell, S

    T. Fennell, S. Bramwell, D. McMorrow, P. Manuel, and A. Wildes, Nat. Phys. 3, 566 (2007)

    2007

  18. [26]

    Therefore, the negative value of h‖ in our model corresponds to the experimentally interest- ing negative tilt of [111] field toward [11¯2] direction

    In order to compare the canted kagome-ice model with py- rochlore spin ice, it is worth noting that h⊥ and h‖ refer to the field strengths along the [111] and [¯1¯12] crystallographic direc- tions of pyrochlore, respectively. Therefore, the negative value of h‖ in our model cor...

  19. [27]

    Chern, P

    G.-W. Chern, P. Mellado, and O. Tchernyshyov, Phys. Rev. Lett. 106, 207202 (2011)

    2011

  20. [28]

    Chern and O

    G.-W. Chern and O. Tchernyshyov, Phil. Trans. R. Soc. A 370, 5718 (2012)

    2012

  21. [29]

    A. S. Wills, R. Ballou, and C. Lacroix, Phys. Rev. B66, 144407 (2002)

    2002

  22. [30]

    Dall and P

    J. Dall and P. Sibani, Comput. Phys. Commun.141, 260 (2001)

    2001

  23. [31]

    A. J. Macdonald, P. C. Holdsworth, and R. G. Melko, J. Phys.: Condens. Matter 23, 164208 (2011)

    2011

  24. [32]

    L. D. Jaubert, M. J. Harris, T. Fennell, R. G. Melko, S. T. Bramwell, and P. C. Holdsworth, Phys. Rev. X 3, 011014 (2013)

    2013

  25. [33]

    Anghinolfi, H

    L. Anghinolfi, H. Luetkens, J. Perron, M. G. Flokstra, O. Sendetskyi, A. Suter, T. Prokscha, P. M. Derlet, S. L. Lee, and L. J. Heyderman, Nat. Commun. 6, 8278 (2015)

    2015

  26. [34]

    Farhan, P

    A. Farhan, P. M. Derlet, L. Anghinolfi, A. Kleibert, and L. J. Heyderman, Phys. Rev. B 96, 064409 (2017)

    2017

  27. [35]

    Zeissler, M

    K. Zeissler, M. Chadha, E. Lovell, L. F. Cohen, and W. R. Branford, Sci. Rep. 6, 30218 (2016)

    2016

  28. [111]

    crystallographic direction on Ho2Ti2O7, yet an unusual critical scattering appears when the field is slightly tilted away from this direction [24]. By using the dipolar spin-ice model with combination of fields, it is shown that the critical scat- tering is ascribable to the lon...

    1908 arXiv

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