## Abstract

Mechanical contacts are crucial to systems in engineering, electronics and biology. The microscopic nature of the contacting surfaces determines how they mesh on the nanoscale. There is thus much interest in methods that can map the actual area of two surfaces in contact—the real contact area—during the loading or unloading phases. We address this problem using an ultrafast optical technique to generate non-equilibrium electrons that diffuse across a nanoscale mechanical contact between two thin gold films deposited on sapphire. We image this process in the contact and near-contact regions to micron resolution *in situ* using transient optical reflectivity changes on femtosecond time scales. By use of a model of the ultrashort-time electron dynamics, we account for an up to ~40% drop in the transient optical reflectivity change on contact. We thereby show how the real contact area of a nanoscale contact can be mapped. Applications include the probing of microelectronic mechanical devices.

## Introduction

Mechanical contacts between solids rely on the meshing of individual asperities on the nanoscale. Such contacts govern the phenomena of friction and lubrication and are exquisitely sensitive to the surface roughness and to the state of the surface^{1}. Elastic and plastic behaviors are often studied with micro- or macroscale indenters^{1,2}, but this does not allow the physics of the deformation process to be studied locally and during loading. One can image nanoindentation processes with nanoscale resolution in a transmission electron microscope, but this is not suited to continuous mapping over the contact area during deformation^{3}. Neither does it provide a measure of the microscopic (i.e. real) area of contact, a quantity of vital importance in understanding adhesion and friction.

The contact area can be directly imaged by ultrasonic, thermal or optical methods^{4,5,6,7,8,9,10}. Ultrasonic methods have two advantages: they may be used to map opaque materials over the whole contact area, and, if very high ultrasonic frequencies are implemented, they potentially allow nanoscale spatial resolution in the through-contact direction^{6,7}. However, it is hard to relate ultrasonic reflection or transmission coefficients quantitatively to the real microscopic contact area. Likewise, mapping with thermal waves involves heat conduction through asperities as well as through the gaps between them, again rendering it difficult to measure this area^{6,7}. Probing the real contact area in transparent solids in static or frictional contact using optical methods is also feasible^{8,9,10}, but these methods are limited by the finite optical wavelength to samples with roughness .

Here we propose a way to map the real contact area of nanoscale contacts: we investigate the mechanical contact between metal-coated materials *in situ* by the use of optically-excited electron transport probed on sub-picosecond time scales. Ultrafast non-equilibrium electron diffusion in metals has been extensively studied by ultrashort-time-scale transient optical reflectivity measurements^{11,12,13,14,15,16,17,18,19,20,21,22} and such techniques have been implemented to image buried metallic layers^{23}. We harness such electrons here to map the mechanical contact between a gold-coated sphere and a gold-coated plane (a Hertzian-contact geometry), offering the crucial advantage of mapping of a nanoscale mechanical contact during loading: for separations greater than angstrom-order, the electrons cannot cross the gaps between the contacting solids and so allow the selective sensing of the real contact area. This sensing we achieve by implementing an analytical model for the diffusion of non-equilibrium electrons through the contacting nano-asperities.

## Results

### Samples and single-point transient reflectivity measurements

Gold films of thickness 37 nm are sputtered onto a sapphire sphere of diameter 2 mm and a sapphire plate of thickness 1 mm. The rms (root mean square) surface roughnesses measured by atomic force microscopy (AFM) are σ_{s} = 1.9 and σ_{i} = 1.6 nm (error ±20%) for the coated plate and sphere, respectively, as shown by typical traces in Fig. 1(b) and (c) and by the corresponding power spectral densities (PSD) in Fig. 1(d) and (e). The sapphire plate is fixed horizontally on a rigid holder, pierced to allow optical access through the plate to the sapphire/gold interface, as shown in Fig. 1(a). The sphere is pressed against the plate, both with vertical (0001) principal crystal axes, using a displacement stage and the load is monitored with a load cell.

We use an optical pump-probe technique with ~200 fs duration pulses of repetition frequency 80 MHz and wavelength 830 nm from a mode-locked Ti:Sapphire laser. The focused pump-beam photons excite electrons in the gold film on the sapphire plate to non-equilibrium states within a distance from the sapphire/gold interface of the order of the optical absorption depth (ζ_{pump} ≈ 12 nm^{24}). These electrons subsequently diffuse into the gold film, probing the mechanical contact when they reach the contacting interface and decay to thermal phonons to produce a transient lattice temperature rise. The optical reflectivity change of the probe beam at wavelength 415 nm (where ζ_{probe} ≈ 17 nm^{24}) is coupled through induced changes in the complex refractive index to the non-equilibrium electron distribution. Image data with ~1 µm spatial resolution is obtained by scanning the coaxial optical spots laterally in two dimensions over the circular contact area.

We first selected the point on the sample corresponding to the center of the mechanical contact and scanned the delay time *t* on changing the load *F*. Figure 1(f) shows the probe relative-reflectivity change *δR*/*R* at *F* = 0 (i.e. before contact with the sample) and at *F* = 0.6 N on loading. A small peak in the reflectivity change is visible centred at *t* = 0, that we believe to be caused by transitions from sharp maxima in the electron density of states^{25} to states ~1 eV above and below the Fermi level. The lifetime of the photoexcited electrons in these states is shorter than 10 fs and they should cause a reflectance change only when the pump and probe pulses temporally overlap. (This represents a precise measure of the *t* = 0 time delay.) We also observe a spike at *t* ≈ 0.9 ps, a time we term τ_{R}, owing to the excitation of non-equilibrium electrons. One can see that the effect of loading is to dramatically reduce this spike height to ~0.6 of that out of contact. (τ_{R} was independent of loading.) At longer times (3–6 ps) there is a smaller rise in *δR*/*R* owing to the transient lattice temperature change Δ*T*_{l} ~ 3 K and residual photoelastic effects. (Small acoustic oscillations after this time allow a determination of the film thickness.) We may ignore these residual photoelastic effects at short times because of the relatively low value of the heat capacity of the electrons^{15}.

We define the spike height at τ_{R} as the difference between the relative reflectivity change at the spike and before the pump-pulse arrival, . For our 3.0 eV probe pulses exciting *d*-state electrons in gold at ~3.075 eV below the Fermi level, the spike height can be considered to be a measure of the non-equilibrium electron quantum-state occupancy (i.e. electron density) of optically-probed state energies *E* ~ 0.075 eV below the Fermi level—see the Supplementary Information. At this probe energy the value of τ_{R} is approximately twice that for the case of infrared probing. (Photon energy 3 eV is larger than the highest value, 2.68 eV, reported for sub-picosecond-resolution experiments on gold^{13}. Transient reflectivity signals at 2.84 eV and 3.06 eV have been reported with ~1.5 ps time resolution^{20}.)

Figure 1(g) shows spike-height data at the center of the contact area when loading up to 1.0 N and then unloading, in steps of 0.2 N for a pristine region of the sample. These curves represent the ratio of the spike heights in and out of contact and we term this quantity the normalized spike height. One can see that loading even by 0.2 N produces a substantial drop in spike height. The relatively low level of hysteresis, below the experimental error, suggests that one can apply models based on elastic deformation to describe the contact mechanics to a first approximation.

### Transient reflectivity imaging over the contact

The ultrafast electronic response can be mapped over the contact area by laterally scanning the pump and probe spot positions. The static probe reflectivity *R* also depends on position and we shall consider *R* first: Figure 2(a) shows an image for *R* for a 56 × 56 µm^{2} region at 1.0 N load (measured simultaneously with *δR*) together with a horizontal cross section through the center of the image. The concentric circles are Newton's rings caused by probe beam interference in the gap between the gold films outside the contact region^{6,7}. The central region inside the rings includes the contact area.

Hertz theory^{1} for the elastic deformation of a sphere of radius *R*_{0} indenting a frictionless half-space gives, for the contact radius *a*, *a*^{3} = 3*FR*_{0}/4*E**, where is the effective modulus of the indenter (*i*) and substrate (*s*) and ν_{i}_{,s} and *E*_{i}_{,s} are Poisson's ratios and Young's moduli, respectively. Outside the contact area, the air gap Δ*d*(*r*) between the sphere and the substrate (i.e. plate) is given as a function of radial distance *r* for *r* > *a* by^{1}

We calculated the Newton's ring patterns using Eq. (1) by the use of parallel-surface multiple-beam reflection theory for the probe beam, taking into account the known refractive indices of gold and sapphire^{24}, but using *E** as a fitting parameter. Figure 2(b) shows a calculated image for *R* at 1.0 N load and its horizontal cross section (solid line) using *E** = 187 ± 5 GPa obtained from an average of a series of measurements at different loads up to 1.0 N. Reasonable agreement in both contrast and spacing is obtained. This value of *E** is 0.8 times that (233 GPa) of a sapphire-sapphire contact^{26} and 2.2 times that (85 GPa) of a more compliant gold-gold contact^{27}. This is as expected given the softening of the contact owing to the gold films^{28,29}. Figure 2(b) also shows the calculated Δ*d* (dotted line) obtained from Eq. (1). The calculated contact areas are shown by the dashed rings in these images.

We now present imaging of the ultrafast electronic response derived from data at *t* = τ_{R} and −1 ps. Figure 2(c) shows normalized spike-height images for the same region as Fig. 2(a) when loading up to 1 N and then unloading, for a pristine region of the sample. As expected from the results of Fig. 1(g), hysteresis in the images for loading and unloading is negligible. The azimuthally-averaged cross sections are shown in the plots below each image (solid lines). Newton's rings for the probe light remain in the normalized quantity *δR*/*R*, because the effect of the probe optical interference in the gap region outside the contact differs for *R* and *δR*^{30}. (Pump light can also cause Newton's rings, but the effect is small here because of the smaller optical absorption depth.)

The Hertz pressure distribution *p*(*r*) = *p*_{0}[1−(*r*/*a*)^{2}]^{1/2} takes a maximum value *p*_{0} = 3*F*/2*πa*^{2} at *r* = 0. The calculated contact areas and pressure distributions are shown respectively by the dashed rings in the images of Fig. 2(c) and the dotted lines in the cross sections. We estimate *a* = 9.3 µm and *p*_{0} = 1.1 GPa at the lowest loads (0.2 N), whereas *a* = 15.9 µm and *p*_{0} = 1.9 GPa at the highest loads (1 N) (with corresponding plate indentations δ_{0} = *a*^{2}/*R*_{0}~85 and 250 nm, respectively). In contrast, the gold film maximum indentations are expected to be much smaller (and in any case small compared to the film thickness) and will be neglected in the analysis in this paper. (We estimate the combined change in film thickness at the center of the contact area at 1 N load owing to elastic and plastic deformations to be ~2 nm.) To apply Hertz theory, the combined surface roughness of the contacting surfaces should also be considered. In our case the parameter for *F* > 0.2 N, so modifications of Hertz theory to account for surface roughness are unnecessary^{1}.

The spatially-resolved data of Fig. 2(c) represents a wide range of pressures, even for a fixed load *F*. For each *F* we sample the data in 1 µm steps in the radial direction for *r* < 0.95*a*. The results for the normalized spike height are plotted in Fig. 3(c) as a function of pressure. Apart from the lower pressures, the value of the normalized spike height is again very close to 0.6.

### Analytical model of the electron diffusion

To understand these results one must first consider the dynamics of transiently heated electrons in gold. A one-dimensional (1D) model of the electron diffusion is appropriate because the electron diffusion length (~100 nm—see below) is much smaller than the optical spot sizes (~1 µm)^{21,22}. The non-equilibrium electron diffusivity is *D*_{e} = κ/*C*_{e}≈1.56 × 10^{−2} m^{2}/s, where κ = 317 W/m K is the equilibrium thermal conductivity and *C*_{e} the electron specific heat^{22}: *C*_{e} = *γT*_{l}, where the constant coefficient γ ≈ 68 J/m^{3}K^{2} and the lattice temperature *T*_{l} ≈ 300 K. The electron diffusion length, , significantly exceeds the probe absorption depth ζ ≈ 17 nm^{24}. For films of thickness , as in our case, it is therefore reasonable when calculating electron diffusion to make the approximation of surface absorption of the photon energy.

We proceed by assuming that the spatiotemporal variation of the non-equilibrium electron density contains a term Ψ(*z*, *t*) that obeys the 1D diffusion equation^{22}. The electron density is obtained by multiplying this term by the temporal form of the solution for homogeneous excitation in the absence of diffusion. For an infinite half-space, this term takes the classical form , where *z* is the perpendicular distance (in the gold) from the excited interface (see Fig. 1)^{22}. For the cases of a single film or two contacting films, a solution can be obtained by considering successive reflections of the diffusion wave front at the film interfaces, where the non-equilibrium electron flux vanishes and its effective reflection coefficient is −1. Electron reflection at the gold/gold interface depends on the contact, so we define an effective reflection coefficient *r*_{f} that lies between 0 (perfect transmission) and −1 (perfect reflection). The appropriate solution for Ψ(*z*, *t*) at the surface (*z* = 0) for the non-contacting case of a film of thickness *d* is in the same form as that of the analogous thermal diffusion problem^{31}:

where is a Jacobi theta function and β(*d*, *t*) = exp[−(2*d*)^{2}/(4*D*_{e}*t*)]. The corresponding equation for the case of two films of thickness *d* in imperfect contact is

This reduces to Eq. (2) when *r*_{f} = −1. The predicted ratio , shown in Fig. 3(a) vs *r*_{f}, varies from the expected value of 1.0 when *r*_{f} = −1 to 0.575 when *r*_{f} = 0. For the simple case of perfect contact one can use Eqs. (2) and (3) to estimate the corresponding normalized spike height at *z* = 0 for two films of thickness *d* = 37 nm at *t* = τ_{R} = 0.9 ps: , in good agreement with experiment in Fig. 3(c) for GPa.

## Discussion

In order to derive the real contact area *S*_{r} at any pressure *p*, one requires a model that relates *S*_{r} to *r*_{f} and to *p*. Assuming plastic flow of non-interacting microscopic gold asperities^{32,33}, the ratio between the real (*S*_{r}) and nominal (*S*_{0}) contact areas can be expressed as a function of *p* by the following empirical equation: *S*_{r}/*S*_{0} = *p*/(*p* + *H*) for loads up to and greater than *H*, where *H* is the Vickers hardness, as shown in Fig. 3(b). (This is an approximation for more complicated theories^{34,35}.) In addition, we expect *r*_{f} to be determined by the ratio between the real and nominal contact areas through *S*_{r}/*S*_{0} = 1−|*r*_{f}| = 1 + *r*_{f}, assuming that the interstitial air gaps prevent electron transport and that asperity-to-asperity contact is perfect. The former assumption is reasonable considering the ~2 nm surface roughness of our gold films (i.e. sub-nm tunneling distances); likewise for the latter assumption, considering that gold does not form an oxide layer. By least-squares fitting of for all data sets using *H* as a fitting parameter, the best fit is obtained with *H* = 0.24 ± 0.10 GPa, as shown by the solid curves in Fig. 3(c). The weighted average of the data in Fig. 3(c) is shown by the dotted curve in Fig. 3(d), giving excellent agreement with the theory (solid curve), including the reproduction of the downward slope. (The weighting was done in inverse proportion to the standard deviations. The variations in the thermal diffusivity of electrons in gold with pressure are estimated not to significantly contribute to the observed changes in spike height. See Ref. 36.) This value of *H* is consistent with that, , reported for gold^{37,38}. Our results thus provide strong evidence that ultrafast electron diffusion can indeed directly map the real (asperity) contact area *S*_{r} in the range from *S*_{r}/*S*_{0} = 0 to the maximum probed value ~0.85.

In conclusion, we have mapped nanoscale-roughness mechanical contacts from transient optical reflectivity changes on femtosecond time scales. By modelling the dynamics of electrons diffusing between contacting metal asperities and using an empirical relation between the real contact area, the hardness and the contact pressure, we demonstrate how the real contact area of a nanoscale contact can be probed *in situ* during loading and unloading. Accessing the real contact area is possible thanks to the insulating spaces between the contacting surfaces, forcing the diffusing electrons to pass only through the meshed nano-asperities. Compared to optical methods for probing the real contact area the present method allows samples with much smaller roughness, down to angstrom-order, to be accessed. At present we are limited to a lateral spatial resolution of ~1 µm, but this could be improved by the use of shorter optical wavelengths or near-field optical methods. In future it would be interesting to probe interfaces between different transparent substrates and metal films; films with greater hardness than gold would, in particular, allow better access to the poor-electrical-contact (low |*r*_{f}|) region. The method can also be extended to Vickers indenters or other types of indenter or to planar contacts. By such direct, local measurements of transient optical reflectivity changes at contacts, this study not only opens the way to the physics of ultrafast electron diffusion across contacting surfaces and inside asperities, with applications in microelectronic devices, but also to the mapping of the real contact area of nanoscale mechanical contacts, invaluable for accessing the underlying mechanisms for adhesion, friction and wear.

## Methods

The frequency-doubled probe beam passes through a delay line and is focused together with the infrared pump beam from below onto the interface between the sapphire plate and the gold film with a ×50 objective lens (numerical aperture 0.35, working distance 18 mm). Pump and probe spot diameters are 1.0 and 1.1 µm (intensity at *e*^{−2}), respectively, with corresponding fluences 11 and 3 J/m^{2} (resulting in steady state temperature rises in and out of contact ~8 and 16 K, respectively).

The optical reflectivity changes of the probe beam are monitored as a function of the time delay *t* between the pump and probe pulses. The pump beam is chopped at a frequency of 1 MHz for synchronous lock-in detection. The probe reflectivity change, coupled to the non-equilibrium electron distribution, varies linearly with the pump fluence up to the value used. Image data is obtained from the difference in the transient reflectivity change at delay times *t* = −1 ps and τ_{R} = 0.9 ps (the spike height). This image data is obtained by scanning the objective lens laterally in two dimensions over the contact area.

The gold films, of thickness 37 nm, are chosen to be reasonably thick compared to the ~10 nm optical absorption depth of the ultrashort light pulses while at the same time being smaller than the ~100 nm electron diffusion depth^{14}.

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## Acknowledgements

We thank Roberto Li Voti for stimulating discussions.

## Author information

### Authors and Affiliations

### Contributions

M.T. and O.B.W wrote the main manuscript text. Y.I., T.D. and M.T. contributed to the measurements. M.T. and Y.I. prepared the samples. V.E.G., M.T., O.M. and O.B.W. contributed to the theory. All authors reviewed the manuscript.

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### Supplementary Information

Supplementary Information: Nanoscale mechanical contacts mapped by ultrashort time-scale electron transport

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### Cite this article

Tomoda, M., Dehoux, T., Iwasaki, Y. *et al.* Nanoscale mechanical contacts mapped by ultrashort time-scale electron transport.
*Sci Rep* **4**, 4790 (2014). https://doi.org/10.1038/srep04790

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DOI: https://doi.org/10.1038/srep04790

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