Scaling in reversible submonolayer deposition

Scaling in reversible submonolayer deposition

T. J. Oliveira and F. D. A. Aarão Reis 1 Departamento de Física, Universidade Federal de Viçosa, 36570-000, Viçosa, MG, Brazil
Instituto de Física, Universidade Federal Fluminense, Avenida Litorânea s/n, 24210-340 Niterói RJ, Brazil
11a) Email address:
b) Email address:
August 29, 2019

The scaling of island and monomer density, capture zone distributions (CZDs), and island size distributions (ISDs) in reversible submonolayer growth was studied using the Clarke-Vvedensky model. An approach based on rate-equation results for irreversible aggregation (IA) models is extended to predict several scaling regimes in square and triangular lattices, in agreement with simulation results. Consistently with previous works, a regime I with fractal islands is observed at low temperatures, corresponding to IA with critical island size , and a crossover to a second regime appears as the temperature is increased to , where is the single bond detachment probability and is the diffusion-to-deposition ratio. In the square (triangular) lattice, a regime with scaling similar to IA with () is observed after that crossover. In the triangular lattice, a subsequent crossover to an IA regime with is observed, which is explained by the recurrence properties of random walks in two dimensional lattices, which is beyond the mean-field approaches. At high temperatures, a crossover to a fully reversible regime is observed, characterized by a large density of small islands, a small density of very large islands, and total island and monomer densities increasing with temperature, in contrast to IA models. CZDs and ISDs with Gaussian right tails appear in all regimes for or larger, including the fully reversible regime, where the CZDs are bimodal. This shows that the Pimpinelli-Einstein (PE) approach for IA explains the main mechanisms for the large islands to compete for free adatom aggregation in the reversible model, and may be the reason for its successful application to a variety of materials and growth conditions.

68.43.Hn, 05.40.-a, 68.35.Fx , 81.15.Aa

I Introduction

The morphology and physical properties of thin films and multilayers are strongly related to the initial stages of their formation ohring ; pimpinelli ; venablesbook . It motivated a large number of works on modeling the submonolayer growth regime etb ; venables1973 ; ratsch , in which a single incomplete layer of adatoms is being formed. These models usually consider a set of fundamental processes (diffusion, aggregation, etc) in order to find activation energies and related quantities for a particular deposition process or with the aim of investigating universal features valid for several materials and techniques.

The simplest models consider irreversible aggregation (IA) of atoms to islands of size larger than a critical value . Rate-equation (RE) approaches predict the scaling of island and monomer densities (, ) etb ; venables1973 for any and show good agreement with simulation data, usually performed for ranging between and etb . The shapes of the island size distributions (ISDs) were proposed by different approximation schemes etb ; venables1973 ; ratsch ; af1995 ; amar2001 ; mb and are still subject of debate. A recent advance by Pimpinelli and Einstein (PE) pe proposed that the capture zone distributions (CZDs) are described by the Wigner surmise (WS) from random matrix theory rmt [the capture zone (CZ) of an island is defined as the area in which a diffusing adatom is more likely to attach to that island than to any other one]. After an initial controversy shi ; li ; pereply , that proposal was supported by simulation results for various island shapes after suitable rescaling tiago2011 , under conditions of high temperatures and low coverages. IA models are expected to model real systems in temperatures sufficiently low to neglect atom detachment from islands, but this condition is not obeyed in many real systems, even at room temperature. For this reason, suitable choices of the size are frequently combined with internal restructuring mechanisms to reconcile experimental data and IA predictions af1995 ; ruiz ; wu ; shiqin ; zheng .

On the other hand, a smaller number of works have addressed scaling properties of models with reversible aggregation (RA) ratschPRL ; ratsch1995 ; bales ; bartelt1995 ; mehl ; furman ; ramadan . Works on square lattices, which simulate metal homoepitaxy, have shown a crossover between IA scaling regimes with and ratsch1995 ; bartelt1995 . Partially reversible models allowing only single-bond detachment were studied using simulations and improved RE approaches and confirmed the crossover scaling between those regimes af1997 ; popescu . The work on triangular lattices, which is related to epitaxy, shows a crossover between regimes with and af1997 ; popescu .

In this paper, we study the scaling properties of island density, CZDs, and ISDs in a model of fully reversible island growth, using numerical simulations in square and triangular lattices and a scaling approach based on RE results for IA models. We consider a canonical bond-counting model of Clarke-Vvedensky cv type, in which the activation energy for an adatom hop to a neighboring site depends only on the number of nearest neighbors at its initial position, with the temperature kept fixed during the growth. It respects detailed balance conditions, in contrast to IA. For a fixed coverage and increasing deposition temperature, the islands evolve from a fractal shape (typical of IA with no island restructuring) to a compact shape dominated by processes of adatom detachment and reattachment, and the island density continuously decrease. The previously studied crossovers of IA regimes are reproduced, but an additional crossover from to in triangular lattices is found. At high temperatures, a nontrivial regime where the island density increases with temperature is observed, with a large density of small clusters coexisting with large compact islands. The Gaussian right tail of CZDs predicted by the PE approach is observed in all regimes for small coverages and sufficiently high temperatures, even when the CZDs are bimodal.

The rest of this work is organized as follows. In Sec. II, we present the RA model and summarize previous theoretical results for IA and RA. In Sec. III, we present the simulation results and a scaling approach in square lattices. In Sec. IV, that discussion is extended to triangular lattices. Sec. V summarizes our results and presents our conclusions.

Ii Basic definitions and theoretical approaches

In the RA model, the adsorbed atoms can occupy sites of a square or triangular lattice, with the maximum of one adatom per site. There is a random flux of atoms per site per unit time. Adsorption is allowed only if the site of incidence is empty, so that a single layer is formed on the substrate lattice. This condition is reasonable for small coverages. The hopping rate of an adatom at a given site is given by (proportional to its surface diffusion coefficient), with the activation energy , where is the number of adatoms in nearest neighbor (NN) sites of , is an energy barrier for surface diffusion of free adatoms, and is the bond energy for each NN.

The parameters , , and were kept fixed in most simulations. The last value is characteristic of epitaxy ratschPRL . Some data were obtained with and in order to confirm general scaling predictions. Broad ranges of temperature were studied, thus the conclusions can be extended to other systems by considering the diffusion-to-deposition ratio of free adatoms as the main model parameter. Due to the large frequency , one typically has , even at low temperatures.

Several values of the bond energy are analyzed, and scaling approaches are facilitated by using the detachment probability (binding factor) . Since is considered throughout this work and the largest experimentally relevant temperatures do not exceed , the condition always applies. It is also important to observe that both and increase with temperature.

Simulations were performed in very large lattices, typically of lateral size , with at least realizations up to coverage for each parameter set. Comparison with results in for the largest coverages and temperatures shows no significant finite-size effect. Standard algorithms were able to provide accurate estimates of densities and distributions up to large values of (however, extensions to the multilayer regime or to models with a larger number of atomistic processes would benefit from special algorithms developed for this class of model shim ).

In the IA models, islands with a number of atoms larger than the critical size are stable. Moreover, islands of size are assumed to have a binding energy . During the deposition process, after a transient regime, islands grow by capture of diffusing adatoms, with negligible formation of new islands. In this steady state, rate-equation theory venables1973 ; etb predicts that the stable island density scales as


and the monomer (free adatom) density scales as




These results assume that the mean capture number of stable islands is independent of the coverage.

Information on the growth dynamics can also be extracted from the probability densities of island size , , and of CZ area , (ISD and CZD, respectively). The ISD follows the scaling form


where is a scaling function, and an equivalent scaling form applies to . Alternatively, scaling with the variance may be used as


This procedure was previously used with IA models tiago2011 and is helpful in other problems, such as scaling of roughness distributions of thin film growth models intrinsic .

The best know approach to predict the shape of CZD in IA is that of PE, which proposes the CZD to be described by the WS

Figure 1: Square lattice islands for (a) , (b) , and (c) . The panels are , , and cuts of systems of size , respectively. The coverages are , , , and from left to right.

where , , is the substrate dimension ( in the present work) and the parameters and are determined by normalization conditions. This proposal follows from the phenomenological argument that the CZD can be extracted from a Langevin equation representing the competition of neighboring islands for adatom aggregation. Several experimental works have already shown agreement of CZDs with the WS, such as growth of para-sexiphenyl islands lorbek ; potocar , deposition with impurities sathiyanarayanan , pentacene island growth with impurities conrad , quantum dot growth on arciprete2010 , and deposition on films groce .

In Ref. tiago2011 , a scaling approach was used to predict the decay of the right tail of the ISD from the Gaussian tail of the CZD (Eq. 6) and the island shape (point, fractal or square).

Iii Square lattice

iii.1 Scaling of island and monomer density

Figs. 1a-c illustrate the island evolution for and temperatures representative of different scaling regimes. Fig. 2a shows the temperature evolution (parametrized by ) of the island density and monomer density for coverage and several values of .

For very low temperatures (), both densities are nearly temperature-independent, and the system behaves as in random sequential adsorption (RSA) without diffusion privman , as discussed in Ref. tiago2012 .

The subsequent low temperature regime, hereafter called regime I, is characterized by the decrease of and with , as shown in Fig. 2a. In this regime, the probability of detachment of an aggregated adatom from an island is negligible during the time interval necessary for the aggregation of a new adatom to its neighborhood. This regime is equivalent to IA with . Using Eq. (1) for fixed coverage, one has

Figure 2: (Color online) Scaled island densities for and several binding energies in the square lattice. Dashed lines indicate local slopes. The insets show scaled monomer densities.

This scaling is highlighted in Fig. 2a. The longer regimes with scaling are observed for ; for (nearly three decades), fits of the data give and , which are consistent with Eq. (7).

The average detachment time of a singly bonded atom is


In a mean-field approach (RE), the time for a free adatom to encounter that aggregated atom is


Regime I is characterized by , so that adatom bonds are effectively stable.

A crossover to a second regime is observed when matches [Eqs. (8) and (9)], as explained in Refs. bartelt1995 ; ratsch1995 ; af1997 (see also Sec. 8.5 of Ref. etb ). A crossover variable is defined as


with in regime I. Regime II begins with . From Eqs. (7) and (10), the crossover scaling for island density and monomer density is


where and are scaling functions. Regime II is effectively characterized by , since detachment of doubly bonded atoms of square islands (size ) occurs in much longer timescales. Thus, for but not very large, Eqs. (1), (2), and (11) give


This result is consistent with a binding energy for the critical island with adatoms.

Fig. 2b illustrates the crossover scaling with the collapse of data in regimes I and II for various . Again, the longest regime with scaling is observed for ; fits of the data for (nearly two decades in ) give and , which are consistent with Eqs. (7) and (12) (see the predicted slopes in Fig. 2b).

For , Fig. 2a shows that the slope of the plot slowly increases in regime II. This occurs because the binding energy becomes negligible at the end of this regime, so that and scale tend to scale only with , as


[the same power laws of Eq. (12) excluding the -dependence]. The same evolution of slopes is observed in all effective IA regimes observed in the RA model (see Sec. IV).

As the temperature increases, a crossover to a new scaling regime is expected by two reasons: rapid detachment of doubly bonded atoms from islands with , which occurs in a characteristic time


or slow atom deposition in the CZ, which occurs in a characteristic time

Figure 3: (Color online) Scaled island densities for and different deposition rates and binding energies in the square lattice. The insets show scaled monomer densities.

In the steady state of IA, [Eq. (15)] is of the same order of [Eq. (9)]. Thus, regime II is expected to end as [Eq. (14)] matches , i. e., when . This defines a second crossover variable as


Crossover scaling follows from Eq. (13) as


Fig. 2c illustrates the crossover scaling for various , with an excellent collapse of data. Some deviations appear for , probably due to scaling corrections. The expected slope before the crossover, predicted by Eq. (13), is also shown in Fig. 2c. The fits of the data for and , in the range (nearly one decade in ), give slopes and , respectively, both close to the theoretical value. This gives additional support to the proposed evolution in regime II, to an -dependent to an -independent scaling.

After the crossover, a fully reversible regime III is attained, completely different from IA. Fig. 2a shows that the island density and the monomer density increase with temperature in this regime, in striking contrast with regimes I and II and all IA models. Fig. 1c shows that it is characterized by a very large density of small islands, mainly isolated adatoms, and a small density of very large islands. As time evolves, these large islands grow at the expense of the small ones, i. e., there is island ripening comsa ; grabow .

In regime III, the density of small islands is much larger than the density of large islands. This is an expected evolution from regime II because decreases with temperature slower than [Eq. (12)]. This trend is expected for any regime with , which gives , and will also be shown in the triangular lattice.

The high-temperature scaling in regime III is only -dependent, with


Indeed, since movement of free adatoms is very fast, only the attachment-detachment dynamics is important to determine the densities.

This steady state regime can be predicted by noting that double bonding is the minimal possible bonding for an island in the square lattice, i. e. at least four atoms of a large island have two bonds. Equating aggregation and detachment rates obtained from Eqs. (9) and (14), we get the above relation for . Since regime III takes place as the evolution of an effective IA regime (also related to lattice structure), where , we obtain the above relation for .

In order to search for possible effects of deposition rate () or amplitude of hopping rates (), Fig. 3 compares the crossover scaling (a) from regimes I to II and (b) from II to III, obtained for and different binding energies . The good data collapses in Fig. 3 show the general validity of the above scaling relations.

iii.2 Capture-zone and island size distributions

Despite the effective IA scaling of regime I, the CZDs usually do not match the WS with () for the values of and temperatures considered here. Fig. 2a shows that regime I typically occurs with . This range is intermediate between low adatom mobility (RSA behavior) and high adatom mobility (PE behavior), thus CZDs show a crossover scaling, as shown in Ref. tiago2012 . Similar crossover is observed in the ISDs. For instance, considering , for we observe simple exponential tails of CZDs (RSA) and for they become Gaussian (PE), but still not collapsing with the WS.

Figure 4: (Color online) Scaled (a) CZDs and (b) ISDs for the energy and temperatures () and (). The insets show the same scaled distributions with squared abscissas. The dashed lines highlight the Gaussian decay of the right tails.
Figure 5: (Color online) (a) Scaled ISDs for , () and several coverages. The inset shows the same data in a log-log scale and the line has slope . (b) Scaled CZDs for the same parameters of (a). The inset shows the same distributions with squared abscissas. The dashed lines highlight the Gaussian decays of the right tails.

The CZDs in regime II are not well fitted by the WS with ( in Eq. 6), probably because this is not a true IA process, as shown in Fig. 4a. However, as the temperature increases, the CZD gets closer to that WS. This occurs considering scaling with the average [Eq. (4)] or with the variance [Eq. (5)]. On the other hand, Fig. 4a shows that the tails of the CZDs are Gaussian, similarly to IA models tiago2011 . This trend fails only for very small because regime II is attained with small and crossover from RSA is present.

The ISD has features similar to those of IA models of compact islands (e. g. square islands), as shown in Fig. 4b: the left tail is high, indicating the presence of a large number of small islands, and the right tail shows a Gaussian decay. As the coverage increases, a crossover to simple exponential decay is observed in the CZDs and ISDs, similarly to the IA models tiago2012 .

Fig. 5a shows ISDs in regime III, with left tails much higher than the peaks, confirming the presence of a large density of free adatoms and small islands. The left tail shows even-odd oscillations characteristic of loose-packed lattices (inset of Fig. 5a). If the small islands were in near-equilibrium conditions, the Walton relation venables1973 ; walton would apply and an exponential decay of the left tail would be observed. However, this is not the case: the inset of Fig. 5a shows an approximately power-law decay, with large exponents that depend on the coverage, which suggests that more complex mechanisms govern the small island dynamics.

In regime III, , thus a small island will probably disappear before a new atom is deposited in its CZ. The concept of CZ as the probable region for deposition of a new atom to be captured by that island becomes irrelevant. Anyway, we also measured the CZDs in that regime and observed that they are bimodal, as shown in Fig. 5b. The first peak corresponds to small islands and the second peak corresponds to the large islands. The bimodal CZDs are completely different from those of IA models, where distortions of the monomodal shapes of ISDs and CZDs appear only for large coverages tiago2012 . As increases, the first peak of the CZD moves to the left (smaller CZs for small islands) and the second one moves to the right (larger CZs for large islands).

A surprising result in the inset of Fig. 5b is that the Gaussian right tail of the CZDs is preserved for low coverages in regime III. Thus, the competition of large islands for the capture of diffusing adatoms is still that predicted by the PE approach in the fully reversible regime. The small islands, which rapidly dissociate into isolated monomers, contribute to maintain the competitive dynamics of the neighboring large islands. The right tails of the corresponding ISDs are also Gaussian, following the trend of compact islands already explained in Ref. tiago2011 .

In experiments, very small islands () may not be detected in microscopy images, except if high resolution techniques are used. If that is the case, the first peak of the bimodal CZDs may be lost, but the Gaussian right tail will be preserved. This may suggest IA behavior in a system with fully reversible dynamics.

Iv Triangular lattice

Fig. 6a shows the -dependence of the island density for various values of . It has the main features of the RA model in the square lattice, including the high temperature crossover to the fully reversible regime, where and increase with . However, some important features of RA are particular of the triangular lattice, as discussed below.

The crossover from a fractal island regime I () to the first regime of compact islands is equivalent to that in the square lattice, occurring when matches and leading to the crossover relations in Eq. (11). This is illustrated in Fig. 6b. The subsequent regime is hereafter called IIa and corresponds to IA with , i. e. with the smaller stable island being a triangle with adatoms, shown in Fig. 7a. From Eq. (11) and the RE equations (1) and (2) for , regime IIa has initial scaling as


This trend is confirmed by the slope of the curves in Fig. 6b after the crossover. Eq. (19) is consistent with a binding energy of the critical island , which is reasonable for a two-adatom island.

As the temperature increases, regime IIa evolves so that the critical island binding energy becomes negligible and island and monomer densities scale as


This evolution parallels that observed in the square lattice.

A crossover to another regime also occurs when the typical aggregation time to an island is of the order of the detachment time of doubly-bonded atoms (Fig. 7a). Matching Eqs. (9) and (14) using (20), we obtain a crossover variable


and crossover scaling as

Figure 6: (Color online) Scaled island densities for and several binding energies in the triangular lattice. Dashed lines indicate local slopes. The insets show scaled monomer densities.

In the square lattice, a similar crossover leads to regime

Figure 7: (Color online) Illustration of stable islands of size (a) () and (b) () on a triangular lattice before (left) and after (right) loosing a particle.

III. However, here it leads to another regime with IA scaling due to the triangular lattice geometry. The reason is that an island with atoms (Fig. 7b), is stable for a time much longer than the island with atoms (Fig. 7a), as will be explained below. Thus a regime with appears when (or ) increases, which is hereafter called regime IIb. Its scaling properties follow by matching the -dependence of Eqs. (1) and (2) for and that in Eq. (22):


Fig. 6c illustrates this crossover scaling. For and , regime IIa (final) is represented approximately by and regime IIb (initial) is represented approximately by , both corresponding to nearly one order of magnitude in . Linear fits of those data provide slopes and , respectively. Both estimates are in good agreement with the predicted slopes shown in Fig. 5c [from Eqs. (20) and (23)].

Figs. 7a and 7b show the islands with and atoms loosing one adatom, which provide the (critical) islands with and , respectively. Both processes of loosing one adatom occur in a characteristic time [Eq. 14]. The island with needs a time to break into two monomers, while the island with needs a time to break into isolated monomers. The addition of these times do not change the order of magnitude of the mean-field rate . However, the stability time of the remaining islands in Figs. 7a and 7b is affected if the recurrence property of two-dimensional random walks is considered.

The probability that a random walker returns to the origin after steps is of order montroll . Thus, the probability that the island with breaks before the return of the detached atom (Fig. 7a) is of order . Analogously, the probability that the island with breaks before the return of the detached atom (Fig. 7b) is of order . Thus, the lifetime of the island with is times larger than the lifetime of the island with . For , a factor has to be introduced in the characteristic time for an island with adatoms to break.

Following these ideas, we incorporate that factor in the mean-field approach by stating that the effective lifetime for the critical island with is


This does not represent a failure of the RE theory, but a suitable form to extend its application. We recall that the RE approach overestimates rates of several processes, as shown in simulation of IA models etb ; zhang ; popescu , but they are overestimated (and characteristic times underestimated) by similar factors, so that the final scaling on , and is correct.

The scaling of and also evolve to -independent forms in regime IIb as the temperature increases:


In regime IIb, the monomer density decreases with temperature slower than island density. Thus, it is expected to be followed by the fully reversible regime III, similarly to the square lattice. Matching with the aggregation time [Eq. (9)] for the regime, the crossover scaling variable is defined as


The crossover scaling is obtained considering Eq. (25):


Fig. 6d illustrates this crossover scaling (again with some deviations in the collapse of due to corrections to scaling).

After this crossover, the high-temperature, fully reversible regime III is observed, with the same basic features of the square lattice. The island and monomer densities scale only with as


thus increasing with temperature. This is also a steady state, nearly deposition independent, where follows from matching of aggregation and detachment times [Eqs. (9) and (24)] and , a relation characteristic of the largest available critical island.

The features of ISDs and CZDs in the triangular lattice are similar to those of the square lattices, including the Gaussian tails observed at high temperatures and extending to the fully reversible regime.

V Conclusion

We analyzed the scaling of island density, CZDs, and ISDs in a model of fully reversible island growth where the activation energy for an adatom hop depends only on the number of NNs at its initial position (Clarke-Vvedensky model). A scaling approach based on rate-equation results for IA models was presented and supported by numerical simulations in square and triangular lattices.

At low temperatures, a regime I with fractal islands is observed, corresponding to IA with critical island size . CZDs and ISDs are usually intermediate between those of RSA (negligible diffusion of free adatoms) and those of PE theory (competition of large islands for rapidly moving adatoms), except for large values of the binding energy , where the regime is extended up to and a nearly Gaussian right tail of CZDs appears.

A crossover to a second regime is always observed as the reduced model parameters satisfy , in agreement with previous works. In the square (triangular) lattice, a regime with scaling similar to IA with () is observed after the crossover. The initial dependence of island density and monomer density with disappears as the temperature increases, so that those quantities scale only with close to the subsequent crossover.

In the triangular lattice, there is a crossover to a third IA regime, with . This is explained by the recurrence properties of random walks in two dimensions, since the detachment times of doubly bonded atoms in islands with and atoms are the same and that feature could not be predicted solely with a mean-field approach.

Although the CZDs shows some deviations from the WS in these regimes with , their right tails are typically Gaussian, indicating that the PE theory is reasonable to represent the competition of large islands for free adatom capture. Exceptions appear for small values of , where those regimes may appear for small .

A final crossover to a fully reversible regime III is observed as () in the square (triangular) lattice. In contrast to IA scaling, this regime is characterized by an increase of the island density and of the monomer density with temperature, for fixed coverage. A large density of small islands coexists with a small density of very large islands. The corresponding ISDs show a high left tail and the CZDs are bimodal. The Gaussian right tails of CZDs and ISDs are also observed, despite the reversible nature of the aggregation, and are explained because the small islands do not change the main mechanisms for the large islands to compete for free adatom aggregation.

These results show that the Gaussian right tails of CZDs are kept in reversible aggregation, as predicted by the PE approach for IA. The same occurs with ISDs. In experiments where the resolution of imaging techniques is not high, detection of small islands may be difficult and even the high temperature regimes may have ISDs and CZDs similar to those of IA. This may explain the success of PE predictions to describe a variety of experimental results, for various materials and growth conditions lorbek ; potocar ; sathiyanarayanan ; conrad ; arciprete2010 ; groce .

The authors acknowledge support from CNPq, FAPEMIG and FAPERJ (Brazilian agencies).


  • (1) M. Ohring, Materials Science of Thin Films - Deposition and Structure, 2nd. ed., Academic Press, 2001.
  • (2) A. Pimpinelli and J. Villain, Physics of Crystal Growth (Cambridge University Press, Cambridge, England, 1998).
  • (3) J. A. Venables, Introduction to Surface and Thin Film Processes (Cambridge University Press, Cambridge, England, 2000).
  • (4) J.W. Evans, P. A Thiel, and M. C. Bartelt, Surf. Sci. Rep. 61, 1 (2006).
  • (5) J. A. Venables, Phyl. Mag. 27, 697 (1973).
  • (6) C. Ratsch and J. A. Venables, J. Vac. Sci. Technol. A 21, S96 (2003).
  • (7) J. G. Amar and F. Family, Phys. Rev. Lett. 74, 2066 (1995).
  • (8) J. G. Amar, M. N. Popescu, and F. Family, Phys. Rev. Lett. 86, 3092 (2001).
  • (9) P. A. Mulheran and J. A. Blackman, Philos. Mag. Lett. 72, 55 (1995); Phys. Rev. B 53, 10261 (1996).
  • (10) A. Pimpinelli and T. L. Einstein, Phys. Rev. Lett. 99, 226102 (2007).
  • (11) M. L. Mehta, Random Matrices (Academic, New York, 2004), 3rd ed; T. Guhr et al, Phys. Rep. 299, 189 (1998).
  • (12) F. Shi, Y. Shim, and J. G. Amar, Phys. Rev. E 79, 011602 (2009).
  • (13) M. Li, Y. Han, and J. W. Evans, Phys. Rev. Lett. 104, 149601 (2010).
  • (14) A. Pimpinelli and T. L. Einstein, Phys. Rev. Lett. 104, 149602 (2010).
  • (15) T. J. Oliveira and F. D. A. Aarão Reis, Phys. Rev. B 83, 201405(R) (2011).
  • (16) R. Ruiz, B. Nickel, N. Koch, L. C. Feldman, R. F. Haglund, Jr., A. Kahn, F. Family, and G. Scoles, Phys. Rev. Lett. 91, 136102 (2003).
  • (17) Y. Wu, T. Toccoli, N. Koch, E. Iacob, A. Pallaoro, P. Rudolf, and S. Iannotta, Phys. Rev. Lett. 98, 076601 (2007).
  • (18) J. Shi and X. R. Qin, Phys. Rev. B 78, 115412 (2008).
  • (19) H. Zheng, M. H. Xie, H. S. Wu, and Q. K. Xue, Phys. Rev. B 77, 045303 (2008).
  • (20) C. Ratsch, A. Zangwill, P. Smilauer, and D. D. Vvedensky, Phys. Rev. Lett. 72, 3194 (1994).
  • (21) C. Ratsch, P. Smilauer, A. Zangwill, and D. D. Vvedensky, Surf. Sci. Lett. 329, L599 (1995).
  • (22) G. S. Bales and A. Zangwill, Phys. Rev. B 55, 1973 (1997).
  • (23) M. C. Bartelt, L. S. Perkins, and J. W. Evans, Surf. Sci. Lett. 344, L1193 (1995).
  • (24) H. Mehl, O. Biham, I. Furman, and M. Karimi, Phys. Rev. B 60, 2106 (1999).
  • (25) I. Furman, O. Biham, J.-K. Zuo, A. K. Swan, and J. F. Wendelken, Phys. Rev. B 62, R10649 (2000).
  • (26) A. Ramadan, F. Picaud, and C. Ramseyer, Surf. Sci. 604, 1576 (2010).
  • (27) J. G. Amar and F. Family, Surf. Sci. 382, 170 (1997).
  • (28) M. N. Popescu, J. G. Amar and F. Family, Phys. Rev. B 58, 1613 (1998).
  • (29) S. Clarke and D. D. Vvedensky, J. Appl. Phys. 63, 2272 (1988).
  • (30) Y. Shim and J. G. Amar, Phys. Rev. B 71, 125432 (2005); J. Chem. Phys. 134, 054127 (2011).
  • (31) T. J. Oliveira and F. D. A. Aarão Reis, Phys. Rev. E 76, 061601 (2007).
  • (32) S. Lorbek, G. Hlawacek, and C. Teichert, Eur. Phys. J. Appl. Phys. 55, 23902 (2011).
  • (33) T. Potocar, S. Lorbek, D. Nabok, Q. Shen, L. Tumbek, G. Hlawacek, P. Puschnig, C. Ambrosch-Draxl, C. Teichert, and A. Winkler, Phys. Rev. B 83, 075423 (2011).
  • (34) R. Sathiyanarayanan, A. BH. Hamouda, A. Pimpinelli, and T. L. Einstein, Phys. Rev. B 83, 035424 (2011).
  • (35) B. R. Conrad, E. Gomar-Nadal, W. G. Cullen, A. Pimpinelli, T. L. Einstein, and E. D. Williams, Phys. Rev. B 77, 205328 (2008).
  • (36) F. Arciprete, M. Fanfoni, F. Patella, A. Della Pia, A. Balzarotti, and E. Placidi, Phys. Rev. B 81, 165306 (2010).
  • (37) M. A. Groce, B. R. Conrad 1, W. G. Cullen, A. Pimpinelli, E. D. Williams, and T. L. Einstein, Surf. Sci. 606, 53 (2012).
  • (38) V. Privman, Colloids Surf. A 165, 231 (2000).
  • (39) T. J. Oliveira and F. D. A. Aarão Reis, Phys. Rev. B 86, 115402 (2012).
  • (40) D. Walton, J. Chem. Phys. 37, 2182 (1962).
  • (41) E. W. Montroll and B. J. West, in Fluctuation Phenomena, edited by E. W. Montroll and J. L. Lebowitz (North-Holland, Amsterdam, 1979).
  • (42) C.-M. Zhang, M. C. Bartelt, J.-M. Wen, C. J. Jenks, J. W. Evans, and P. A. Thiel, Surf. Sci. 406, 178 (1998).
  • (43) K. Morgenstern, G. Rosenfeld, E. Laegsgaard, F. Besenbacher, and G. Comsa, Phys. Rev. Lett. 80, 556 (1998).
  • (44) M. Zinke-Allmang, L. C. Feldman, and M. H. Grabow, Surf. Sci. Rep. 16, 377 (1992).
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