Critical exponents and scaling invariance in the absence of a critical point
The paramagnetic-to-ferromagnetic phase transition is believed to proceed through a critical point, at which power laws and scaling invariance, associated with the existence of one diverging characteristic length scale – the so called correlation length – appear. We indeed observe power laws and scaling behavior over extraordinarily many decades of the suitable scaling variables at the paramagnetic-to-ferromagnetic phase transition in ultrathin Fe films. However, we find that, when the putative critical point is approached, the singular behavior of thermodynamic quantities transforms into an analytic one: the critical point does not exist, it is replaced by a more complex phase involving domains of opposite magnetization, below as well as the putative critical temperature. All essential experimental results are reproduced by Monte-Carlo simulations in which, alongside the familiar exchange coupling, the competing dipole-dipole interaction is taken into account. Our results imply that a scaling behavior of macroscopic thermodynamic quantities is not necessarily a signature for an underlying second-order phase transition and that the paramagnetic-to-ferromagnetic phase transition proceeds, very likely, in the presence of at least two long spatial scales: the correlation length and the size of magnetic domains.
pacs:75.70.Kw, 05.70.Fh, 64.60.Cn, 75.30.Kz, 75.70.Ak
Our understanding of the ferromagnetic phase transition foresees the appearance of a finite, spatially uniform spontaneous (i.e. occurring in zero applied magnetic field) magnetization as the temperature is lowered below a well-defined critical (Curie) temperature Landau (). Strictly speaking, however, a finite three-dimensional body (i.e. a body extending over sufficiently large but finite lengths in all three spatial directions) lacks a finite uniform magnetization at any temperature Griffiths (), as a result of the dipole-dipole interaction, which, albeit weak, frustrates the tendency to ferromagnetism inherent to the exchange interaction Arrott (); Houches (). Thus, the dipole-dipole interaction leads necessarily to a situation of “avoided critical point” Kivelson (), where the phase transition proceeds via a yet not fully elucidated and probably not universal mechanism Kivelson (); Bra (); Abanov (); Barci_PRB_2009 (); Cannas_PRB_2004 (); Schmalian-Wolynes_PRL2000 (); Note (). At present, both the theoretical and experimental behavior of the various thermodynamic quantities in the vicinity of such an avoided critical point are uncertain. Here we demonstrate, on one side, the validity of conventional notions like critical exponents and scaling hypothesisLandau () in the vicinity of such an avoided critical point, implying the existence of a correlation length governing the phase transition. On the other side, we also establish that, when the putative critical point is approached, the non-analytic behavior transforms into an analytic one. Simultaneously, we observe that the paramagnetic-to-ferromagnetic phase transition proceeds within a background of spatially nonuniform magnetization. This observation implies that the typical period of modulation – established by the competition between exchange and dipole-dipole interaction and characterizing the phase with nonuniform magnetization – persists below as well as above the putative critical temperature, alongside the correlation length.
The paramagnetic-to-ferromagnetic phase transition investigated in this work occurs in
ultrathin Fe films grown at room temperature by molecular-beam epitaxy onto the (001)
surface of a Cu single crystal (see Ref. Saratz_PhD_2009, for details). The system
has macroscopic lengths within a plane but finite thickness perpendicular to the plane (typically between 1.6 and 2.0 atomic monolayers (ML)). It is magnetized perpendicularly to the plane, so that it has the right symmetry to realize the famous Onsager critical point OnsagerYang () of the two-dimensional (2D) Ising model. However, as shown in
Ref. Biskup, , it also suffers the very same
frustration foreseen for finite three-dimensional bodies so that the paramagnetic-to-ferromagnetic phase transition is associated with the appearance of stripes and/or bubble domains of opposite magnetization rather than with the formation of a spatially uniform spontaneous magnetization Abanov (); Seul_Science_1995 (); Allenspach_PRL_1992 (); Saratz_PRL_2010 (); Saratz_PRB_2010 (); Qiu (); Back_Nature_13 (); Cannas_PRB_2011 (); Debell (); Diaz-Mendez_PRB_2010 (); Pighin_PRB_2007 (). Accordingly, the transition falls into the category of transitions with “avoided critical point”.
We have followed three strategies: On one side an experimental one, consisting in performing magneto-optical Kerr effect (MOKE) Moke () measurements of the macroscopic, spatially averaged magnetization as a function of temperature and external magnetic field applied perpendicularly to the film. Technically speaking, MOKE measures a signal which is proportional to the average magnetization Moke (). Here we use the character “” to identify the measured quantity, which is accordingly given in arbitrary units. In a second step, the measurement of macroscopic thermodynamic quantities was complemented with spatially resolved magnetic imaging – performed with SEMPASaratz_PRB_2010 () – aimed at measuring the evolution of the local magnetization during the phase transition, with submicrometer spatial resolution. The complementary use of MOKE and SEMPA microscopy to define the phase diagram of the Fe films investigated in this work is pictorially sketched in Fig.1. Finally, we explored the possibility of realizing the scaling hypothesis in Monte-Carlo simulations of a 2D Ising model, with spins on a lattice and interacting via the familiar exchange interaction – which promotes ferromagnetic order – and dipolar interaction. The latter, albeit weak, is long ranged and in films magnetized perpendicularly to the plane frustrates the tendency to ferromagnetism. In the presence of the dipolar interaction, it is not a priori clear whether any scaling behavior – explicit in the 2D Ising model with pure exchange interaction – is left behind, nor in which region of the parameter space such scaling might be found.
iii.1 Scaling plots
Magnetization curves are plotted as a -family of isochamps in Fig.2. The magnetic field was swept with a frequency varying between and Hz. -curves measured at fixed temperature within this range of frequencies coincide: we assume that we are observing properties related to thermodynamic equilibrium. At higher frequencies we have detected a substantial dynamical component and the results of these studies will be reported in a separate paper. A color code, indicated along the vertical bar, is used for the values of . We distinguish two extreme sets of -curves. On the right-hand side those corresponding to larger values of , taken in a state of uniform magnetization. They show the familiar behavior of -curves separating out with increasing magnetic field and are suggestive of a conventional underlying critical point becoming more and more “avoided” with increasing applied magnetic field (this is an example of trivially “avoided critical point” Kivelson ()). On the left-hand side the family of curves corresponding to low : while the temperature is increased the average magnetization abruptly drops to almost zero as the system enters the state of static modulated order, observed directly with SEMPA (not reported here). Those images indicate that the magnetization within the domains is still large and therefore the vanishing of (global magnetization) below 300 K for small applied fields is entirely due to the cancellation of finite opposite values of the local magnetization within the domains. We point out, however, that our distinction between “high” and “low” magnetic field curves is based on our imaging of the spatial distribution of the magnetization: the macroscopic thermodynamic quantity itself does not contain, at first glance, any specific information which could be used to classify the set of -curves.
The scaling hypothesis Landau () states that the equation of state can be simplified to a one variable relation , provided the rescaled variables and are used, being the so called reduced temperature. In conventional ferromagnets is the critical temperature at which, e.g., the critical isochamp (order parameter) vanishes. The critical exponent is defined via the asymptotic behavior of the critical isochamp near , i.e. . In our system this curve does not exist because domains form spontaneously as soon as some sizable magnetization develops locally, leading to cancellation of the global magnetization. As a consequence, cannot be located in a standard way, nor can be determined directly. The critical exponent is defined via the asymptotic behavior of the critical isotherm , which – streactly speaking – does not exist either. However, the conventional lore of scaling (Ref. Landau, , p.485) in the critical or near critical region indicates practical ways to extrapolate values for , and using experimental -data originating within the high-temperature, non-zero field region of the parameter space, as discussed in Appendices A and B.
iii.2 Phase diagram
Using the values of , and determined experimentally, the data of can be represented in a scaling plot versus : The data points that collapse onto the same master curve obey the equation of state of a conventional ferromagnet in the vicinity of . Therefore, “collapsed” and “non-collapsed” points can be reported in the proper location of the plane to define the phase diagram. In the scaling plot of Fig.2 (bottom), locations with higher density of data points can be recognized by inspection. Using an ad-hoc software, we marked the low-density points – which we consider as “non-collapsed” – in gray, while the high-density points – which we consider as “collapsed” – were left in their original color (vertical bar in Fig.2). The gray (non-collapsed) data and the black (collapsed) ones are subsequently transferred into their place in the plane, Fig.3, where they appear inside, respectively outside, a bell-shaped region marked in gray. To represent the phase diagram in Fig.3 the variable is used. Notice that many reddish color-coded points appear in the lower left-hand section of the scaling plot Fig.2 (bottom). They correspond to high temperatures and low applied magnetic fields and they are scattered because of noise, resulting in a small density. Despite this, we consider them as “collapsed”, because they are spread along the continuation of the scaling function of the 2D Ising model (the dashed line in Fig.2 (bottom)). The bell-shaped region starts on the left with the boundary line marking the transition from (static) modulated-to-uniform phase, recorded by direct SEMPA imaging of the spatial distribution of the magnetization. It continues beyond the range of temperature and magnetic fields where a static modulation of order is observed and even beyond , that is above . Evidently, the static magnetic domains Saratz_PRL_2010 () imaged with SEMPA represent only a small portion of the ferromagnetic transition.
Remarkably, the singular behavior of expected for a conventional ferromagnet while is approached gives way to an analytic behavior within the “gray zone”. In particular, the versus dependence for low magnetic fields is perfectly linear within the “gray” zone, i.e. at sufficiently low magnetic fields a singular behavior, characterized by some non-linear versus relationship, does not develop. It appears, therefore, that the non-analytic behavior is precisely suppressed when the putative critical point is approached.
iii.3 Griffiths-Widom representation
An alternative way with respect to Fig.2 (bottom) to express the equation of state of a ferromagnet is the Griffiths-Widom representation Griffiths-Widom ():
with . In Fig.4 the same data points shown in Fig.2 (bottom) are plotted in this representation with the same color coding. Particularly clear is how gray points deviate from scaling for the data plotted in the inset (). In the main frame the non-collapsed, gray points decorate the colored line of clearly collapsed points up to . For larger values of , the main line broadens as well: these are the high temperature, low-field “noisy” data points already discussed in relation to Fig.2. In the Griffiths-Widom representation data collapsing is realized over forty orders of magnitude with respect to the -variable and eighty orders of magnitude with respect to the variable . The theoretical scaling function given in Ref. Gaunt_JPhysC_1970, for the unfrustrated 2D Ising model is plotted as a green dashed line. Colored, collapsed points follow this curve very well up to (note the remarkable agreement in the inset).
iii.4 Monte-Carlo simulations
We consider the Hamiltonian Pighin_PRB_2007 ()
where the spins are defined on a square lattice with sites and periodic boundary conditions (Ewald sums technique was used to handle them). The first term in Eq. (2) represents the short-range exchange interaction (the sum runs over all pairs of nearest-neighboring sites). The second term represents the long-range dipolar interaction in the Ising limit, the corresponding sum running over all pairs of distinct sites on the lattice. The third term represents the Zeeman energy. The Hamiltonian in Eq. (2) is far from describing ultrathin Fe films on Cu(100) in detail. However, it is considered to build a model Hamiltonian capturing realistically competing interactions and the avoided critical point. Accordingly, it has been found to display a variety of modulated phases Debell (); Diaz-Mendez_PRB_2010 (); Pighin_PRB_2007 (); Cannas_PRB_2006 () within some region of the parameter space, even for those moderate values of the ratio where Monte-Carlo simulations are practicable footnote1 (). In this particular study we have explored the phase diagram outside this region, with the aim of searching for some residual scaling behavior. In a first step we have determined a limiting field above which the system is in a spatially uniform state, within the temperature range considered by the simulation. was determined from the behavior of the average spin polarization as a function of temperature for fixed values of , according to a zero-field-cooled–field-cooled (ZFC-FC) protocol footnote2 (). In a second step we have computed isochamps during the heating part of the ZFC-FC cycle, shown on the top of Fig.5 for and . The spreading of the isochamps with different values of the magnetic field is similar to the experimental one reported in the top of Fig.2. In a third step we attempted scaling plots, trying to bring the isochamps to collapse onto one single curve. It turned out that collapsing could be indeed realized for (colored in the bottom of Fig.5) and a significant departure from collapsing was observed for (gray points corresponding to ), i.e. inside the region of the phase diagram where nonuniform magnetization appears. For building the scaling plots of Fig.5 we used the known 2D Ising critical exponents, but the value for the putative critical temperature , required to build the reduced temperature , cannot be read out in an obvious way from the set of isochamps of Fig.5. We found, for a practicable set of values, that the best data collapse could be realized assuming a transition temperature given in the inset of Fig.5 (bottom) as a function of . Remarkable about this temperature is that it can be expressed as the transition temperature for the “pure” 2D Ising model subtracted by a value which corresponds to about (see Inset of Fig.5 (bottom)). We recall that, within a simple mean-field approach, the presence of the dipolar interaction in a uniformly magnetized state reduces the transition temperature by an amount corresponding to about ! The picture emerging from Fig.5 is in line with the experimental outcome and underlines the realization of scaling and power laws in a situation where the critical point is avoided.
The familiar description of a second-order phase transition foresees that at
sufficiently large temperatures the free-energy density in the variable (average magnetization) has a minimum at (Fig.6, top). When the temperature is lowered below a critical value , the graph of acquires a flat portion (Fig.6, top) between two limiting values defining a situation of spontaneously broken symmetry with spatially uniform magnetization . The present paper is in contrast to this picture because it finds that the flat portion is replaced by a minimum of at for any temperature (Fig.6, bottom).
Notice that we are not the first to point out the difficulty of translating the familiar description of second-order phase transitions Landau () to the paramagnetic-to-ferromagnetic transition Griffiths (); Arrott (). But the present results pinpoint some essential elements of the “gray zone” replacing the critical point which were not recognized explicitly yet:
) the recovery of the familiar properties of scaling and power laws, albeit outside the
gray zone and ) the persistence above the putative critical temperature of the phase of the magnetic-domain patterns, accessible to spin-sensitive scanning probe techniques only below and when
domains are static (on the time scale of a specific scanning-probe experiment).
It is important to mention at this point the vast literature Poki (); Amn () describing the cross-over from the exchange controlled criticality to the dipolar-controlled criticality within a very narrow temperature range in the vicinity of the critical point. Notice that the cross-over considered in this literature preserves the critical point (albeit with slightly modified critical exponents), in contrast to our observations. However, the cross-over scenario refers to a situation of uniform spontaneous magnetization which is actually forbidden for finite three-dimensional bodies. We can, in principle, envisage special situations where a uniform magnetization is possible, such as the infinite-volume limit underlying the cross-over scenarios Poki (); Amn (), but also an inefficient domain nucleation that keeps the body in a metastable state of uniform magnetization, or some very particular shapes (not covered by Ref. Griffiths, ) which energetically penalize the formation of domains. However, the true absence of any domain, both below as well as above the putative critical point, must be verified specificallyAA1 (), as these situations must be regarded as exceptional while the rule is rather a “gray zone”, i.e. an avoided critical point. Unfortunately, it is very difficult to establish, on the base of experimental and theoretical data related to macroscopic thermodynamic quantities alone, the extent of the gray zone AA2 ().
In summary, the recovering of the scaling hypothesis outside the “gray region” means, on one side, that scaling properties and critical exponents, referring to macroscopic thermodynamic quantities, are not necessarily a proof of the existence of a critical point. On the other side, their emergence in a situation of avoided criticality, where the phase transition actually might even be a purely dynamical one Note (), sets some well-defined boundaries on future realistic models of the ferromagnetic phase transition (and of second-order phase transitions in general). These models will have to take into account the presence of (at least) two mesoscopic spatial scales: the correlation length, whose divergence at the putative critical point is an essential ingredient for the current understanding of critical phenomena, and the dipolar-induced period of modulation characterizing the phase with domain patterns.
Acknowledgments – We thank Thomas Bähler for technical assistance, G. M. Graf, A. Giuliani, O. V. Billoni and S. Ruffo for helpful discussions as well as the Swiss National Science Foundation, ETH Zurich, and CONICET (Argentina) for financial support.
Appendix A Experimental determination of
One useful property of a conventional second-order phase transition is that the plot of the magnetic susceptibility
as a function of the temperature has a maximum at a temperature that approaches as approaches zero Change-Lee (). Figure 7 (top) shows the susceptibility of the “pure” (i.e. without dipolar interactions) 2D Ising model computed by means of Monte-Carlo simulations. For any the maximum value of is finite but – as expected – it is higher the weaker the fields are.
Notice that the true approach of to may not necessarily be linear in , as pointed out in Ref. Change-Lee, , but our numerical simulations (bottom of Fig.7) show that a linear extrapolation of toward gives a fairly accurate estimate of .
From the experimental data we obtained the by first treating the raw data with a Savitzky-Golay finite-impulse-response smoothing filter implemented in MATLAB. After filtering, the derivative could readily be obtained. In Fig.8 (top) some of the resulting susceptibility curves are shown for selected values of . The experimental is plotted at the bottom of Fig.8. This graph, in contrast to the one of the “pure” 2D Ising model, shows two distinct regimes, depending on the range of . We discuss first the low temperature regime. When cooling in weak enough fields, the system first enters the “gray zone”, (see the phase diagram in Fig.2 of the main document), without displaying any anomaly in the susceptibility in correspondence of this transition. Upon further cooling a re-entrant transition from the patterned to the uniform phase is encountered Saratz_PRL_2010 (); Saratz_PRB_2010 (); port (): this second transition is accompanied by a sharp maximum in the susceptibility (abrupt increase of the magnetization). This type of maxima – highlighted by a blue dashed line in Fig.8 (bottom) – when extrapolated to leads to a temperature at which the sample consists of very large stripes carrying opposite but almost saturated values of the magnetization Saratz_PRL_2010 (); Saratz_PRB_2010 (); port (). Above this temperature, the sample keeps the modulated order up , where domains become mobile but the magnetization within them is still substantial. Accordingly, must be above . On the other side, for larger fields (the right-hand side portion of the graph) the “gray zone” is never entered and the system is in a uniform state: for larger was therefore taken to extrapolate towards a putative . Several linear fittings were performed by choosing different ranges of the field between T and T. The different fittings produced the family of red lines (bottom of Fig.8) from which the error on the was estimated. The experimental , for this particular sample, is K. Notice that the extrapolated lies within the cross-over range (K) , in which the “blue-line” types of maxima transform into the “red-line” types of maxima.
Appendix B Experimental determination of and
The critical exponent can be deduced from the experimentally determined values of the exponents and , using the relation . The exponent determines the magnetization in the region of weak fields (Eq. 148.8. in Ref. Landau, ) according to
The exponent determines the magnetization in the region of strong fields according to the relation
(see Eq. 148.10 in Ref. Landau, ). The notion of “weak” and “strong” field is, of course, dependent on which temperature interval is addressed.
In Fig.9 we plot versus for different values of , with the color code indicating the values of (see horizontal scale in the inset). At sufficiently high temperatures, a region of the graph emerges where all curves for different magnetic fields almost collapse onto one single straight line, and thus fulfill the scaling properties required by Eq. (1) for the quantity . The negative of the slope of the resulting straight line is the sought-for exponent . Several linear fittings were performed for fixed fields ranging from T to T; these independent determinations of are shown in the inset.
After averaging, for K we obtain , with the error given by the standard deviation of the mean.
As consistency check, the whole procedure was repeated varying the value of . The standard deviation of the mean values of goes through a minimum in the range (K) , which is, accordingly, the range where the “best collapsing” of the -curves is realized. When is varied in this interval, ranges from 1.7 to 1.9.
The versus plot of Fig.10 in the temperature range (K) , reveals a low-field region where the curves saturate to an almost constant vale, indicating the linearity of versus for weak fields. In the strong-field region the graphs are observed to almost collapse onto a single straight line, the slope of which amounts to , consistently with Eq. 2. From these slopes fitted for different in the appropriate regime of Fig.10 we estimate .
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