Physics:Spin glass

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Short description: Disordered magnetic state
Schematic representation of the random spin structure of a spin glass (top) and the ordered one of a ferromagnet (bottom)
Amorphous SiO2
Glass (amorphous SiO2)
Crystalline SiO2)
Quartz (crystalline SiO2)
The magnetic disorder of spin glass compared to a ferromagnet is analogous to the positional disorder of glass (left) compared to quartz (right).

In condensed matter physics, a spin glass is a magnetic state characterized by randomness, besides cooperative behavior in freezing of spins at a temperature called 'freezing temperature' Tf.[1] In ferromagnetic solids, component atoms' magnetic spins all align in the same direction. Spin glass when contrasted with a ferromagnet is defined as "disordered" magnetic state in which spins are aligned randomly or without a regular pattern and the couplings too are random.[1]

The term "glass" comes from an analogy between the magnetic disorder in a spin glass and the positional disorder of a conventional, chemical glass, e.g., a window glass. In window glass or any amorphous solid the atomic bond structure is highly irregular; in contrast, a crystal has a uniform pattern of atomic bonds. In ferromagnetic solids, magnetic spins all align in the same direction; this is analogous to a crystal's lattice-based structure.

The individual atomic bonds in a spin glass are a mixture of roughly equal numbers of ferromagnetic bonds (where neighbors have the same orientation) and antiferromagnetic bonds (where neighbors have exactly the opposite orientation: north and south poles are flipped 180 degrees). These patterns of aligned and misaligned atomic magnets create what are known as frustrated interactions – distortions in the geometry of atomic bonds compared to what would be seen in a regular, fully aligned solid. They may also create situations where more than one geometric arrangement of atoms is stable.

Spin glasses and the complex internal structures that arise within them are termed "metastable" because they are "stuck" in stable configurations other than the lowest-energy configuration (which would be aligned and ferromagnetic). The mathematical complexity of these structures is difficult but fruitful to study experimentally or in simulations; with applications to physics, chemistry, materials science and artificial neural networks in computer science.

Magnetic behavior

It is the time dependence which distinguishes spin glasses from other magnetic systems.

Above the spin glass transition temperature, Tc,[note 1] the spin glass exhibits typical magnetic behaviour (such as paramagnetism).

If a magnetic field is applied as the sample is cooled to the transition temperature, magnetization of the sample increases as described by the Curie law. Upon reaching Tc, the sample becomes a spin glass and further cooling results in little change in magnetization. This is referred to as the field-cooled magnetization.

When the external magnetic field is removed, the magnetization of the spin glass falls rapidly to a lower value known as the remanent magnetization.

Magnetization then decays slowly as it approaches zero (or some small fraction of the original value—this remains unknown). This decay is non-exponential and no simple function can fit the curve of magnetization versus time adequately.[2] This slow decay is particular to spin glasses. Experimental measurements on the order of days have shown continual changes above the noise level of instrumentation.[2]

Spin glasses differ from ferromagnetic materials by the fact that after the external magnetic field is removed from a ferromagnetic substance, the magnetization remains indefinitely at the remanent value. Paramagnetic materials differ from spin glasses by the fact that, after the external magnetic field is removed, the magnetization rapidly falls to zero, with no remanent magnetization. The decay is rapid and exponential.[citation needed]

If the sample is cooled below Tc in the absence of an external magnetic field and a magnetic field is applied after the transition to the spin glass phase, there is a rapid initial increase to a value called the zero-field-cooled magnetization. A slow upward drift then occurs toward the field-cooled magnetization.

Surprisingly, the sum of the two complicated functions of time (the zero-field-cooled and remanent magnetizations) is a constant, namely the field-cooled value, and thus both share identical functional forms with time,[3] at least in the limit of very small external fields.

Edwards–Anderson model

This is similar to the Ising model. In this model, we have spins arranged on a [math]\displaystyle{ d }[/math]-dimensional lattice with only nearest neighbor interactions. This model can be solved exactly for the critical temperatures and a glassy phase is observed to exist at low temperatures.[4] The Hamiltonian for this spin system is given by:

[math]\displaystyle{ H = -\sum_{\langle ij\rangle} J_{ij} S_i S_j, }[/math]

where [math]\displaystyle{ S_i }[/math] refers to the Pauli spin matrix for the spin-half particle at lattice point [math]\displaystyle{ i }[/math], and the sum over [math]\displaystyle{ \langle ij\rangle }[/math] refers to summing over neighboring lattice points [math]\displaystyle{ i }[/math] and [math]\displaystyle{ j }[/math]. A negative value of [math]\displaystyle{ J_{ij} }[/math] denotes an antiferromagnetic type interaction between spins at points [math]\displaystyle{ i }[/math] and [math]\displaystyle{ j }[/math]. The sum runs over all nearest neighbor positions on a lattice, of any dimension. The variables [math]\displaystyle{ J_{ij} }[/math] representing the magnetic nature of the spin-spin interactions are called bond or link variables.

In order to determine the partition function for this system, one needs to average the free energy [math]\displaystyle{ f\left[J_{ij}\right] = -\frac{1}{\beta} \ln\mathcal{Z}\left[J_{ij}\right] }[/math] where [math]\displaystyle{ \mathcal{Z}\left[J_{ij}\right] = \operatorname{Tr}_S \left(e^{-\beta H}\right) }[/math], over all possible values of [math]\displaystyle{ J_{ij} }[/math]. The distribution of values of [math]\displaystyle{ J_{ij} }[/math] is taken to be a Gaussian with a mean [math]\displaystyle{ J_0 }[/math] and a variance [math]\displaystyle{ J^2 }[/math]:

[math]\displaystyle{ P(J_{ij}) = \sqrt{\frac{N}{2\pi J^2}} \exp\left\{-\frac N {2J^2} \left(J_{ij} - \frac{J_0}{N}\right)^2\right\}. }[/math]

Solving for the free energy using the replica method, below a certain temperature, a new magnetic phase called the spin glass phase (or glassy phase) of the system is found to exist which is characterized by a vanishing magnetization [math]\displaystyle{ m = 0 }[/math] along with a non-vanishing value of the two point correlation function between spins at the same lattice point but at two different replicas:

[math]\displaystyle{ q = \sum_{i=1}^N S^\alpha_i S^\beta_i \neq 0, }[/math]

where [math]\displaystyle{ \alpha, \beta }[/math] are replica indices. The order parameter for the ferromagnetic to spin glass phase transition is therefore [math]\displaystyle{ q }[/math], and that for paramagnetic to spin glass is again [math]\displaystyle{ q }[/math]. Hence the new set of order parameters describing the three magnetic phases consists of both [math]\displaystyle{ m }[/math] and [math]\displaystyle{ q }[/math].

Under the assumption of replica symmetry, the mean-field free energy is given by the expression:[4]

[math]\displaystyle{ \begin{align} \beta f ={} - \frac{\beta^2 J^2}{4}(1 - q)^2 + \frac{\beta J_0 m^2}{2} - \int \exp\left( -\frac{z^2} 2 \right) \log \left(2\cosh\left(\beta Jz + \beta J_0 m\right)\right) \, \mathrm{d}z. \end{align} }[/math]

Sherrington–Kirkpatrick model

In addition to unusual experimental properties, spin glasses are the subject of extensive theoretical and computational investigations. A substantial part of early theoretical work on spin glasses dealt with a form of mean-field theory based on a set of replicas of the partition function of the system.

An important, exactly solvable model of a spin glass was introduced by David Sherrington and Scott Kirkpatrick in 1975. It is an Ising model with long range frustrated ferro- as well as antiferromagnetic couplings. It corresponds to a mean-field approximation of spin glasses describing the slow dynamics of the magnetization and the complex non-ergodic equilibrium state.

Unlike the Edwards–Anderson (EA) model, in the system though only two-spin interactions are considered, the range of each interaction can be potentially infinite (of the order of the size of the lattice). Therefore, we see that any two spins can be linked with a ferromagnetic or an antiferromagnetic bond and the distribution of these is given exactly as in the case of Edwards–Anderson model. The Hamiltonian for SK model is very similar to the EA model:

[math]\displaystyle{ H = -\sum_{i\lt j} J_{ij} S_i S_j }[/math]

where [math]\displaystyle{ J_{ij}, S_i, S_j }[/math] have same meanings as in the EA model. The equilibrium solution of the model, after some initial attempts by Sherrington, Kirkpatrick and others, was found by Giorgio Parisi in 1979 with the replica method. The subsequent work of interpretation of the Parisi solution—by M. Mezard, G. Parisi, M.A. Virasoro and many others—revealed the complex nature of a glassy low temperature phase characterized by ergodicity breaking, ultrametricity and non-selfaverageness. Further developments led to the creation of the cavity method, which allowed study of the low temperature phase without replicas. A rigorous proof of the Parisi solution has been provided in the work of Francesco Guerra and Michel Talagrand.[5]

The formalism of replica mean-field theory has also been applied in the study of neural networks, where it has enabled calculations of properties such as the storage capacity of simple neural network architectures without requiring a training algorithm (such as backpropagation) to be designed or implemented.[6]

More realistic spin glass models with short range frustrated interactions and disorder, like the Gaussian model where the couplings between neighboring spins follow a Gaussian distribution, have been studied extensively as well, especially using Monte Carlo simulations. These models display spin glass phases bordered by sharp phase transitions.

Besides its relevance in condensed matter physics, spin glass theory has acquired a strongly interdisciplinary character, with applications to neural network theory, computer science, theoretical biology, econophysics etc.

Infinite-range model

This is also called the "p-spin model".[7] The infinite-range model is a generalization of the Sherrington–Kirkpatrick model where we not only consider two spin interactions but [math]\displaystyle{ r }[/math]-spin interactions, where [math]\displaystyle{ r \leq N }[/math] and [math]\displaystyle{ N }[/math] is the total number of spins. Unlike the Edwards–Anderson model, similar to the SK model, the interaction range is still infinite. The Hamiltonian for this model is described by:

[math]\displaystyle{ H = -\sum_{i_1 \lt i_2 \lt \cdots \lt i_r} J_{i_1 \dots i_r} S_{i_1}\cdots S_{i_r} }[/math]

where [math]\displaystyle{ J_{i_1\dots i_r}, S_{i_1},\dots, S_{i_r} }[/math] have similar meanings as in the EA model. The [math]\displaystyle{ r\to \infty }[/math] limit of this model is known as the random energy model. In this limit, it can be seen that the probability of the spin glass existing in a particular state, depends only on the energy of that state and not on the individual spin configurations in it. A gaussian distribution of magnetic bonds across the lattice is assumed usually to solve this model. Any other distribution is expected to give the same result, as a consequence of the central limit theorem. The gaussian distribution function, with mean [math]\displaystyle{ \frac{J_0}{N} }[/math] and variance [math]\displaystyle{ \frac{J^2}{N} }[/math], is given as:

[math]\displaystyle{ P\left(J_{i_1\cdots i_r}\right) = \sqrt{\frac{N^{r-1}}{J^2 \pi r!}} \exp\left\{-\frac{N^{r-1}}{J^2 r!} \left(J_{i_1 \cdots i_r} - \frac{J_0 r!}{2N^{r-1}}\right)\right\} }[/math]

The order parameters for this system are given by the magnetization [math]\displaystyle{ m }[/math] and the two point spin correlation between spins at the same site [math]\displaystyle{ q }[/math], in two different replicas, which are the same as for the SK model. This infinite range model can be solved explicitly for the free energy[4] in terms of [math]\displaystyle{ m }[/math] and [math]\displaystyle{ q }[/math], under the assumption of replica symmetry as well as 1-Replica Symmetry Breaking.[4]

[math]\displaystyle{ \begin{align} \beta f ={} &\frac{1}{4}\beta^2 J^2 q^r - \frac{1}{2}r\beta^2 J^2 q^r - \frac{1}{4}\beta^2 J^2 + \frac{1}{2}\beta J_0 r m^r + \frac{1}{4\sqrt{2\pi}}r\beta^2 J^2 q^{r-1} +{} \\ &\int \exp\left(-\frac{1}{2}z^2\right) \log\left(2\cosh\left(\beta Jz \sqrt{\frac{1}{2}rq^{r-1}} + \frac{1}{2}\beta J_0 r m^{r-1}\right)\right)\, \mathrm{d}z \end{align} }[/math]

Non-ergodic behavior and applications

A thermodynamic system is ergodic when, given any (equilibrium) instance of the system, it eventually visits every other possible (equilibrium) state (of the same energy). One characteristic of spin glass systems is that, below the freezing temperature [math]\displaystyle{ T_\text{f} }[/math], instances are trapped in a "non-ergodic" set of states: the system may fluctuate between several states, but cannot transition to other states of equivalent energy. Intuitively, one can say that the system cannot escape from deep minima of the hierarchically disordered energy landscape; the distances between minima are given by an ultrametric, with tall energy barriers between minima.[note 2] The participation ratio counts the number of states that are accessible from a given instance, that is, the number of states that participate in the ground state. The ergodic aspect of spin glass was instrumental in the awarding of half the 2021 Nobel Prize in Physics to Giorgio Parisi.[8][9][10]

For physical systems, such as dilute manganese in copper, the freezing temperature is typically as low as 30 kelvins (−240 °C), and so the spin-glass magnetism appears to be practically without applications in daily life. The non-ergodic states and rugged energy landscapes are, however, quite useful in understanding the behavior of certain neural networks, including Hopfield networks, as well as many problems in computer science optimization and genetics.

Self-induced spin glass

In 2020, physics researchers at Radboud University and Uppsala University announced they had observed a behavior known as self-induced spin glass in the atomic structure of neodymium. One of the researchers explained, "...we are specialists in scanning tunneling microscopy. It allows us to see the structure of individual atoms, and we can resolve the north and south poles of the atoms. With this advancement in high-precision imaging, we were able to discover the behavior in neodymium, because we could resolve the incredibly small changes in the magnetic structure." Neodymium behaves in a complex magnetic way that had not been seen before in a periodic table element.[11][12]

History of the field

A detailed account of the history of spin glasses from the early 1960s to the late 1980s can be found in a series of popular articles by Philip W. Anderson in Physics Today.[13][14][15][16][17][18][19]

See also


  1. [math]\displaystyle{ T_c }[/math] is identical with the so-called "freezing temperature" [math]\displaystyle{ T_f }[/math]
  2. The hierarchical disorder of the energy landscape may be verbally characterized by a single sentence: in this landscape there are "(random) valleys within still deeper (random) valleys within still deeper (random) valleys, ..., etc."


  1. 1.0 1.1 Mydosh, J A (1993). Spin Glasses: An Experimental Introduction. London, Washington DC: Taylor & Francis. pp. 3. Template:Isbnt. ISBN 0748400389. 
  2. 2.0 2.1 Joy, P A; Kumar, P S Anil; Date, S K (7 October 1998). "The relationship between field-cooled and zero-field-cooled susceptibilities of some ordered magnetic systems". J. Phys.: Condens. Matter 10 (48): 11049–11054. doi:10.1088/0953-8984/10/48/024. Bibcode1998JPCM...1011049J. 
  3. Nordblad, P; Lundgren, L; Sandlund, L (February 1986). "A link between the relaxation of the zero field cooled and the thermoremanent magnetizations in spin glasses". Journal of Magnetism and Magnetic Materials 54–57 (1): 185–186. doi:10.1016/0304-8853(86)90543-3. Bibcode1986JMMM...54..185N. 
  4. 4.0 4.1 4.2 4.3 Nishimori, Hidetoshi (2001). Statistical Physics of Spin Glasses and Information Processing: An Introduction. Oxford: Oxford University Press. pp. 243. ISBN 9780198509400. 
  5. Michel Talagrand, Mean Field Models for Spin Glasses Volume I: Basic Examples (2010)
  6. Gardner, E; Deridda, B (7 January 1988). "Optimal storage properties of neural network models". J. Phys. A 21 (1): 271. doi:10.1088/0305-4470/21/1/031. Bibcode1988JPhA...21..271G. 
  7. Mézard, Marc; Montanari, Andrea (2009). Information, physics, and computation. Oxford graduate texts. Oxford: Oxford university press. ISBN 978-0-19-857083-7. 
  8. Geddes, Linda (2021-10-05). "Trio of scientists win Nobel prize for physics for climate work". 
  9. "Scientific Background for the Nobel Prize in Physics 2021". 5 October 2021. 
  10. Umut Kamber; Anders Bergman; Andreas Eich; Diana Iuşan; Manuel Steinbrecher; Nadine Hauptmann; Lars Nordström; Mikhail I. Katsnelson et al. (May 29, 2020). "Self-induced spin glass state in elemental and crystalline neodymium". Science 368 (6494). doi:10.1126/science.aay6757. Retrieved 29 May 2020. 
  11. Radboud University Nijmegen (May 28, 2020). "New 'Whirling' State of Matter Discovered: Self-Induced Spin Glass". 
  12. Philip W. Anderson (1988). "Spin Glass I: A Scaling Law Rescued". Physics Today 41 (1): 9–11. doi:10.1063/1.2811268. Bibcode1988PhT....41a...9A. 
  13. Philip W. Anderson (1988). "Spin Glass II: Is There a Phase Transition?". Physics Today 41 (3): 9. doi:10.1063/1.2811336. Bibcode1988PhT....41c...9A. 
  14. Philip W. Anderson (1988). "Spin Glass III: Theory Raises its Head". Physics Today 41 (6): 9–11. doi:10.1063/1.2811440. Bibcode1988PhT....41f...9A. 
  15. Philip W. Anderson (1988). "Spin Glass IV: Glimmerings of Trouble". Physics Today 41 (9): 9–11. doi:10.1063/1.881135. Bibcode1988PhT....41i...9A. 
  16. Philip W. Anderson (1989). "Spin Glass V: Real Power Brought to Bear". Physics Today 42 (7): 9–11. doi:10.1063/1.2811073. Bibcode1989PhT....42g...9A. 
  17. Philip W. Anderson (1989). "Spin Glass VI: Spin Glass As Cornucopia". Physics Today 42 (9): 9–11. doi:10.1063/1.2811137. Bibcode1989PhT....42i...9A. 
  18. Philip W. Anderson (1990). "Spin Glass VII: Spin Glass as Paradigm". Physics Today 43 (3): 9–11. doi:10.1063/1.2810479. Bibcode1990PhT....43c...9A. 


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