Whether an impacting droplet1 sticks or not to a solid surface has been conventionally controlled by functionalizing the target surface2,3,4,5,6,7,8 or by using additives in the drop9,10. Here we report on an unexpected self-peeling phenomenon that can happen even on smooth untreated surfaces by taking advantage of the solidification of the impacting drop and the thermal properties of the substrate. We control this phenomenon by tuning the coupling of the short-timescale fluid dynamics—leading to interfacial defects upon local freezing—and the longer-timescale thermo-mechanical stresses—leading to global deformation. We establish a regime map that predicts whether a molten metal drop impacting onto a colder substrate11,12,13,14 will bounce, stick or self-peel. In many applications, avoiding adhesion of impacting droplets around designated target surfaces can be as crucial as bonding onto them to minimize waste or cleaning. These insights have broad applicability in processes ranging from thermal spraying12,15 and additive manufacturing16,17,18,19 to extreme ultraviolet lithography20.
We release molten tin droplets of millimetric size (R = 0.95 ± 0.03 mm) from a nozzle, such that they hit a target surface with moderate velocity (v = 1.9 ± 0.1 m s−1, see Methods). Figure 1a shows a comparison between the deposition and subsequent solidification of a droplet (initial temperature Td,0 = 240 °C) onto a silicon wafer (top) and a glass slide with ∼200 times lower thermal conductivity (bottom). While the solidified droplet (or splat) sticks to the glass surface, it unexpectedly detaches from the silicon surface: we call this phenomenon ‘self-peeling’ (see Fig. 1a (top) at 3 and 100 ms, the increasing air gap between droplet and surface being a manifestation of this self-peeling).
Two main differences can be observed at this stage. First, interferometric profilometry (see Fig. 1b) confirms that the bottom of the droplet impacting on glass is perfectly flat, while it has a nearly spherical bending curvature κ = 16 m−1 when deposited on silicon. Second, both bottom interfaces show a texture21 formed by annular regions spaced by air ridges (insets of Fig. 1b) that act as interfacial defects. Their number is much higher for silicon than for glass. The striking contrasts in bending and defect density suggest that a balance between thermally induced stress and adhesion determines whether or not a droplet can self-peel upon solidification.
To unravel the competing phenomena, we study the dynamics of the impact using high-speed photography through a transparent surface (see Supplementary Movie 2). Immediately upon contact, micrometre-sized annular air ridges are being trapped. Along the splat radius, their height increases up to a few micrometres, and their width up to tens of micrometres (as measured by profilometry). We also extract the distance d between ridges and the contact line velocity vCL from Supplementary Movie 2, and find that the characteristic timescale τ = d/vCL to form these ridges increases radially. Figure 2a shows that the typical timescale for ridge formation, 10 μs, is much faster than the typical time for the droplet to completely crash22, 2R/v ∼ 1 ms. These observations suggest that the number of ridges is set by a local competition between heat extraction—leading to solidification—and fluid motion—opposing it through local shear, mixing, and convection (see first stage of sketch in Fig. 2c). We propose that at short timescales (<1 ms, top row sketch of Fig. 2c), while the contact line of molten tin spreads outwards, a thin liquid layer in the immediate vicinity of the surface cools down until it forms a solid crust. At that moment, the contact line pins, while the liquid above keeps spreading on a thin air film squeezed underneath. Upon renewed touchdown of the liquid, a small air ridge remains trapped, forming the above-mentioned defect structure. Another example of the fluid–thermal coupling is the existence of a texture-free central patch (see Figs 1b and 2a and Supplementary Fig. 3) due to a vertical flow of hot liquid (acting as a heat supply) and a contact line with diverging23 velocity that prevents air ridge formation at early time.
Once the droplet has completely spread out, ∼1 ms—forming this thin crust with air ridges that act as defects—it makes a flat pancake that solidifies (middle row of sketch in Fig. 2c) within longer timescales (∼10 ms in the example shown in Fig. 2b). Bending of the droplet can be tracked in real time (Supplementary Movie 2 and Fig. 2b) by measuring the spatio-temporally varying air gap δbetween droplet and surface using reflection interference microscopy (RIM, see Methods). It is observed that the droplet already starts peeling-off at the time of solidification (middle row of sketch in Fig. 2c) and that its curvature is created during the homogenization of the vertical thermal gradient (up to a few ∼100 ms, see bottom row of sketch in Fig. 2c). If the bending stress σκ overcomes adhesion stress σA, the splat self-peels. Thus, microtexture formation and thermally induced bending stress are strongly separated in time, yet their combined effect determines the self-peeling behaviour of the splat. Finally, the drop cools down and thermalizes with the surroundings without noticeable change in curvature.
To predict the delamination or sticking outcome of an impacting molten droplet for a given set of parameters we assume that the droplet and surface are two semi-infinite bodies that are brought into contact12,24. In this model (see details in Supplementary Information), droplet interfacial temperature Td,int arises as the natural parameter, is time-invariant and given by:
Here, Td,0 and Ts,0 are initial droplet and substrate temperature respectively, the other relevant droplet and substrate properties being conductivity k, density ρ, and heat capacity cp. It follows from this parameterization, as shown in black in Fig. 3a, that effusivity ei (i = s for substrate, i = d for droplet) is the relevant thermal property governing our system: for large effusivity ratio es/ed ≫ 1, heat from the droplet can be easily transported away from the interface (Td,int ≈ Ts,0), while for small effusivity ratio es/ed ≪ 1, heat is trapped at the interface (Td,int ≈ Td,0). The phase change can be taken into account using the more refined Schwarz model (in red, see Supplementary Information for details). As a consequence of the release of latent heat, this model yields a slightly higher interfacial temperature, in very good agreement with infrared thermography measurements (see Supplementary Information including Supplementary Fig. 2). The Schwarz model still predicts time-invariant Td,int and similar dependency towards the key parameters. Since it has no analytical solution, the simpler conduction model remains extremely valuable to predict parameters’ dependency. We deliberately ignore more complex dynamics due to coupling of fluid dynamics, solid mechanics, and heat transfer—for example, liquid convection inside the splat, overall splat cooling by convection, and delamination that changes the thermal boundary condition—that can be addressed only by using a full numerical simulation.
Predicting interfacial temperature is key since it is expected to play a major role both on defect density (related to adhesion25, see Fig. 4c) and thermal stresses (related to bending26,27). As droplet interfacial temperature Td,int decreases, it is easier to solidify the spreading liquid, so we expect defect distance d to decrease as well. Indeed, since Fig. 3a predicts a lower interfacial temperature for silicon wafer compared to glass, we should observe an increased defect density for the silicon substrate, as confirmed in Fig. 1b. It can be deduced from this enhanced defect density on silicon that its adhesion to the splat should be in turn lower (compared to glass). Regarding bending, if we approximate the splat by a free thin metal disk with a linear through-the-thickness temperature gradient ΔT, thin plate theory26 predicts a spherical curvature κ ∼ α(ΔT/h) due to thermal expansion of the tin upon cooling (α, linear expansion coefficient, h, thickness). Maximum thermal gradient across the solid splat—setting the maximum bending that we can observe eventually—occurs at the time of full solidification (upon which the model is still valid, see Methods). If we assume ΔT ∼ Tmelt − Td,int and use κ as an indirect measurement of the thermal stresses, we expect the stress to increase with decreasing interfacial temperature. This is confirmed in Fig. 3b when varying either Ts,0 (red markers) or Td,0 (blue markers) and calculating the corresponding Td,int using the Schwarz model. Symmetrically, for sufficiently high Td,int, the curvature drops to zero as adhesion stress σA overcomes thermally induced stress σκ and the splat sticks to the surface (squares). For even higher interfacial temperature the droplet remains liquid and bounces off (star). Based on these observations, we define a critical initial surface temperature Ts,0∗, or critical initial droplet temperature Td,0∗, for which the droplet interface remains above the solidification temperature and the whole droplet remains liquid. In this case the Schwarz model converges to the conduction model—with analytical solution in equation (1)—and introducing Td,int = Tmelt leads to:
With these few ingredients, we can now summarize in Fig. 4a, b the overall impact outcome in a three-region phase diagram: a regime of interfacial freezing (or interfacial melting, not treated experimentally) where the drop undergoes phase change (blue areas) and two more familiar regimes consisting of a liquid droplet never freezing (red area: Td,0 > Td,0∗) and a solid droplet never melting (pale blue area, see Supplementary Information). Within the interfacial freezing regime, as we approach Td,0∗, adhesion stresses increase—due to lower defect density—at the same time that thermal stresses decrease—due to smaller temperature gradients. As a consequence, there will be a crossover point below which the splat self-peels (σκ > σA) and above which it sticks (σA > σκ). To validate our model, we performed experiments with varying surface temperature (Fig. 4a) and surface effusivity (Fig. 4b), and recorded the possible deposition behaviour: liquid recoil (stars), sticking (squares) and self-peeling (circles). The corresponding results highlight the ubiquitous presence of self-peeling and liquid recoil with a sticking region in between, and validate the choice of interfacial temperature as a parameter allowing a simple parameterization of our system.
Although the broadening of the sticking regime above Td,0∗ surpasses the parameterization, we experimentally characterize this phenomenon by studying the existence of a central re-molten patch (see glass, fused silica and central region of quartz and zinc selenide in Fig. 4c). Its texture is made of bubbles resulting from the contraction of the air ridges trapped in the interfacial crust. Its presence is the signature of the transient formation of an initial crust (see Supplementary Movie 3) that is subsequently re-melted, typically hundreds of microseconds later. This phenomenon is restricted to a region close to Td,0∗ (see Fig. 4c and Supplementary Figs 4 and 5). Indeed, if the initial droplet temperature is too high, Td,0 ≫ Td,0∗, the crust never forms (recoil regime) and if it is too low, Tmelt < Td,0 ≪ Td,0∗, the liquid flowing on top of the crust does not have enough energy to re-melt it (interfacial freezing regime). In between, extra sticking behaviour exists (extending the initial prediction above Td, 0∗) due to the transient formation of a crust not able to completely re-melt, particularly at the outermost radial portion of the splat where there is an absence of hot liquid above it. As a consequence, just before full recoil can happen, we systematically observe de-wetting starting from the centre leading to liquid accumulation on the pinned ring as seen for glass in Fig. 4c.
We introduce a new approach to control droplet adhesion to the substrate based on thermal properties of the solid, rather than surface functionalization. Even if a droplet of molten liquid impacting on a surface can initially stick, self-peeling can occur upon solidification and result in detachment. We identify that the coupling of early-time defect formation to late-time solid mechanics governs this phenomenon. By using a simple model based on the interfacial temperature, and balancing adhesion with bending stresses, we are able to define and capture the possible outcome regimes: bouncing (liquid or solid), sticking and self-peeling. We expect that this approach can be extended to other liquids28,29,30 (water, wax, thermoplastics) and other freezing applications where adhesion must be controlled, such as powder metallurgy, inkjet printing and de-icing.
Droplet impact experiments.
To create molten tin droplets, tin shot (Sigma-Aldrich) is heated to a temperature above Tmelt = 231.9 °C in a stainless steel cavity surrounded by a resistive heater31. The liquid tin temperature is measured near the nozzle and is varied between 240 and 400 (±1) °C. Droplets are shot through a sapphire nozzle (D = 885 μm ring jewel bearing from SwissJewel Company) using a pressure pulse generated by a solenoid valve (ASCO 411 Series, 15VDC 2.0 W). The pulse is tuned using a pulse generator (Quantum Composers Plus 9518), varying the pressure from 65 to 75 psi and pulse width from 13 to 17 ms, to obtain a single jetted droplet of millimetric size, R = 0.95 ± 0.03 mm. The temperature of the droplet at impact Td,0 is assumed to be similar to the liquid tin temperature; cooling during flight due to flow convection is estimated to be smaller than 5 °C. The thermal properties of tin are shown in Supplementary Table 2. To prevent tin oxide skin formation, the droplets are formed within a closed chamber that is purged with nitrogen32. We verified that droplets are spherical upon impact (in contrast to oxidized droplets that show a characteristic tail). The droplets spread to a pancake-like shape since their impact Weber number We = ρRv2/σ = 48 (ρ: liquid density; σ: surface tension) is well below the splashing threshold.
We use a series of target surfaces to vary the surface effusivity es over two orders of magnitude, from 103 to 105 Ws1/2 m−2 K−1. Crystalline optical materials are obtained from Crystran, copper from McMaster Carr (super conductive 101 that was polished by Princeton Scientific Corp. to an r.m.s. roughness of 2.6 nm), and glass slides from Fisher Scientific. Since roughness is at maximum a few nanometres for all surfaces, we expect splat–substrate adhesion to arise from dispersive adhesion. Since the drop gradually detaches from the perimeter inwards, bending stresses originating from differential shrinking between top and bottom of the splat (as for splats with mechanical interlocking bonded central area33) are expected to be negligible. Since all substrates have a crystalline form (except the copper), they have a high surface energy—of the order of 1 J m−2 (versus 30 mJ m−2 for low-energy surfaces such as plastics and composites). Adhesion between splat and substrate is set by surface energy and the area of contact. Since the latter varies strongly between surfaces, due to strong variations of defect density at the splat–substrate interface, we expect it to be the dominant parameter, while relatively small variations in surface energy can be neglected.
Thermal properties of all target surfaces are shown in Supplementary Table 1. In addition to surface effusivity, the surface temperature Ts,0 is varied between 25 and 200 (±1) °C. Changing surface properties es and Ts,0 gives a more controlled mechanism to change the interfacial temperature (equation (1)) than changing the temperature Td,0 of the droplet. (Indeed, the droplet being liquid, its thermal properties are strongly coupled with fluid dynamic properties. A variation of the liquid temperature is expected to directly impact interfacial temperature, but may indirectly affect it as well through the modification of the flow dynamics). Surface thickness L is chosen such that the characteristic timescale for diffusion τd = L2/αdiff > 100 ms is larger than the timescale for droplet solidification (αdiff: thermal diffusivity of the material). This implies that all target surfaces except diamond can be considered as semi-infinite bodies for the purpose of interfacial temperature calculations. It should be noted that our tin splats have a τd ≈ 10 ms, after which finite effects start to play a role. Most importantly, we can consider our semi-infinite body model as a good candidate up to the freezing time (order 10 ms) when the maximum cross-thickness temperature gradient—that determines the final splat bending curvature—is set.
The dynamics of droplet impingement and solidification are recorded using high-speed photography (Photron Fastcam SA1.1) at up to 20,000 frames per second. Recording from the side yields the evolution of the overall drop shape and an estimate of the bulk solidification time. Recording from the bottom yields the dynamics of defect formation and lift-off; this requires a transparent surface (thus excluding silicon and copper). In addition, observing the dynamics of lift-off relies on interference of reflections from the target surface and the droplet that yield a typical fringe pattern (see Supplementary Movie 2) from which the air gap between droplet and surface can be deducted. We use reflection interference microscopy (RIM set-up: see ref. 34) with a wavelength λ = 572 μm, leading to a vertical spacing of approximately λ/4 = 143 μm between subsequent fringes. The contrast of the RIM technique is a function of the reflection coefficients of the tin and the target surface; in our set of surfaces, zinc selenide gives the highest contrast, and is used for demonstration in Supplementary Movie 2 and Fig. 2. The depth of view is set by both λ/4 and the lateral resolution of the microscope objective, which limits visibility to interface slopes of ≲1° (ending of data points in Fig. 2b).
‘Self-peeling’ splats can be gently brushed-off from the target substrate using a cotton tip, which leaves their bent shape undisturbed. Their equilibrium curvature is visualized by means of an optical profilometer using white light (Zygo) or laser (Keyence VK-x250 Laser Microscope) interferometry. The obtained shape is fitted with a spherical cap to extract the curvature κ. Sphericity is confirmed visually and by agreement (within typically 7%) of κ fitted for either the full splat or the centre region (r = 1.5 mm). Deviations are mainly attributed to slight folding of splats, or slight flattening in the stickier central patch. An average curvature is determined based on four to six repeated experiments per experimental condition.
The data that support the plots within this paper and other findings of this study are available from the corresponding author upon request.
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We acknowledge funding from Alstom. J.d.R. acknowledges a Rubicon fellowship from the Netherlands Organisation for Scientific Research (NWO). We thank F. Mugele from the University of Twente for using their reflection interference microscopy set-up.
The authors declare no competing financial interests.
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de Ruiter, J., Soto, D. & Varanasi, K. Self-peeling of impacting droplets. Nature Phys 14, 35–39 (2018). https://doi.org/10.1038/nphys4252
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