# Coalescence of immersed droplets on a substrate

## Abstract

The dynamics of droplets on substrates has a strong impact on microfluidic systems ranging from commercially available lab-on-chip systems to state of the art developments in open microfluidics. Coalescence of micro and nano droplets on a substrate has been studied extensively, but in previous studies the focus has been on the interface movement. Here, we use computer simulations to investigate coalescence of droplets immersed in another liquid, in an inertia-dominated regime and also investigate the droplet’s internal flow field. It is found that qualitatively the dynamics is similar to coalescence in air, with the same self-similar growth laws. We here point out the ambiguity in the scaling argument for droplets of , that shows itself in the velocities. We show that droplets with a contact angle below exhibit a self-similar velocity field, and the corresponding scaling laws are identified. For drops of , however, it is shown that the velocity field has a more intricate structure that is beyond the usual scaling arguments invoked for coalescence.

###### pacs:

47.55.df, 47.55.D-, 47.85.mb∎ \SendSettingsToPgf

## 1 Introduction

Commercially available microfluidic devices generally consist of closed channels. These are of advantage in order to prevent evaporation and allow to pump fluids by applying a pressure difference between inflow and outflow boundaries. However, keeping the channels clean is a serious problem due to clogging. Open microfluidic systems are an alternative route, where droplets and rivulets are confined to chemically patterned substrates containing wetting surface domains on a less wetting substrate DOERFLER (); DOERFLER-24 (); DOERFLER-25 (); DOERFLER-26 (); DOERFLER-27 (); DOERFLER-28 (). While flow in chemical channels cannot be induced by pressure differences, capillary forces due to wettability gradients DOERFLER-29 (), or electrowetting DOERFLER-33 () are a possible alternative. Another practical possibility are shear forces induced by a covering immiscible fluid DOERFLER-41 (). The advantage of this approach is also that it prevents evaporation and contamination, e.g. with dirt or dust. In microfluidic systems and in open systems in particular, the separation and coalescence of micro and nano droplets is a common phenomenon. However, it occurs not just in microfluidics, but in various situations, such as cloud formation, film formation TenNij00 () or inkjet printing KarRie13 (); LiuMeiWan14 (); ThoTipJue14 (). While sessile droplets with a contact angle of are comparable to freely suspended droplets, sessile droplets of different contact angles are omnipresent and can have a significantly altered behaviour, as we show in this work. Many different phenomena are found in this process, like jumping of the coalescing droplets LiuGhiFen14 (), a transition from coalescence to noncoalescence KarHanFerRie14 (); KarRie13 (), variations in the meniscus shape BilKin05 () and resulting behavior HerLubEdd12 (), mixing SunMac95 (); ZhaObeSwa15 () or the growth rate dependence of the meniscus on the contact angle SuiMagSpe13 (); GroSteRaa13 (). Furthermore, a large interest in droplets and bubbles submerged in a liquid exists LohZha15 (); BerPosGun84 (); BhuWanMaa08 (); BorDamSch07 (). Often experiments on droplets are performed submerged BaiWhi88 (), in order to reduce the influence of gravity, to scale diffusion SuNee13 (); DucNee06 () or in order to study altered friction behavior Raa04 (); SchHar11 ().

Of particular interest is the initial coalescence dynamics, just after the drops are brought into contact. The two drops become connected by a small liquid bridge that rapidly grows in time (Fig. 1). This rapid motion is due to the large curvature that induces a very large (negative) Laplace pressure, driving the liquid into the bridge between the two drops. This process has for example been studied extensively for freely suspended drops PauBurNag11 (); PauBurNag211 (); EggLisSto99 (); DucEggJos03 (); AarLekGuo05 (); SprShi14 (). Here we concentrate on drops on a substrate, which further complicates the geometry of the coalescence process RisCalRoy06 (); NarBeyPom08 (); LeeKanYoo12 (); HerLubEdd12 (); EddWinSno13-2 (); SuiMagSpe13 (); MitMit15 (). An important observation is that the dominant direction of the flow is oriented from the center of the drops towards the bridge, such that the relevant scaling laws can be inferred from quasi-two-dimensional arguments RisCalRoy06 (); NarBeyPom08 (); HerLubEdd12 (); EddWinSno13-2 (); SuiMagSpe13 (). Interestingly, for inertia-dominated coalescence it was shown that droplets of a contact angle behave differently from those of a lower contact angle. Even small deviations from lead to a faster growth of the bridge height in time, which can be described in terms of scaling laws. In particular, the inertial coalescence changes from for , to a power law for smaller angles EddWinSno13-2 (); SuiMagSpe13 (). In both cases the shape of the liquid bridge exhibits a self-similar dynamics, but with different horizontal and vertical scales when the contact angle reaches .

In this paper we focus on the coalescence of sessile drops immersed in another liquid, as it is relevant in open microfluidics. This has been addressed in the viscous regime MitMit15 (), for which both the drops and the surrounding fluid were highly viscous. Here we perform lattice Boltzmann simulations in the inertial regime and define the outer fluid to be of the same density as the coalescing droplets. We investigate how the bridge dynamics changes as a function of the contact angle and, to the best of our knowledge, for the first time investigate whether self-similar behavior can be identified in the velocity field. A detailed comparison to experiments EddWinSno13-2 () of drops in air is provided, pointing out similarities and differences with respect to immersed droplets. The paper starts with a description of the lattice Boltzmann method, and we pay particular attention to the initiation of the coalescence (Sec. 2). The central results are presented in Sec. 3 and the paper closes with a discussion in Sec 4.

## 2 Simulation Method

### 2.1 The lattice Boltzmann method

The coalescence of droplets is a quasi 2D problem RisCalRoy06 (); HerLubEdd12 (); EddWinSno13-2 (), so in favor of numerical speed we choose to perform our simulations in 2D. To investigate the coalescence of droplets on a substrate DOERFLER (), we use the lattice Boltzmann method (LBM) Raa04 (); Suc01 (); BenSucSau92 () in a D2Q9 configuration Sri14 (); QiaYueSuc95 (), that can be described by

(1) |

where is a probability distribution function of particles with mass of component at position and time , following the discretized velocity direction . The left hand side of (1) is the streaming step, where the probability distribution functions of the fluid is distributed to the surrounding lattice sites. The timestep , the lattice constant and the mass of this process are chosen unity for simplicity. On the right hand side of (1), the collision step, these distributions relax towards an equilibrium distribution

(2) |

on a timescale determined by the relaxation time . The relaxation time is directly proportional to the kinematic viscosity as . For simplicity is chosen unity here. Forces can be added by shifting the equilibrium distribution function and thereby implicitly adding an acceleration ShaChe94 (). Multiple components may coexist on every lattice site. Via forces, these can interact with each other. Here we follow the method described by Shan and Chen ShaChe94 ()

(3) |

These interaction forces cause the separation of fluids and a surface-tension . Here we restrict ourselves to two fluids and refer to them as “red” and “blue” fluids. The width of fluid interfaces and the resulting surface tension are governed by the interaction strength parameter , which is chosen as for all shown simulations. This results in a surface tension of . Our choice of parameters implies that the viscous length scale is comparable to the lattice unit . The resulting scale for the coalescence is thus much larger than the viscous length, ensuring we are in the inertial regime of coalescence EggLisSto99 (); PauBurNag11 (); EddWinSno13-2 ().

In this setup the droplets sit on a horizontal flat substrate. The horizontal no slip boundary sites defining the substrate are modified to include a pseudo-density SchHar11 () equal to the average of the surrounding fluid sites. Interactions as described in (3), with interaction parameters and cause a contact angle HuaHauTho07 (); SchHar11 (). In equation (3) and act in place of the interaction strength parameter and scale the absolute interaction force of the wall on the fluids, but defines the contact angle HuaHauTho07 (). The parameters are chosen as to minimize absolute forces.

Using full slip boundaries to effectively mirror the system at the symmetry axis, the computational domain and therefore computational cost is halved. The computational costs have to be considered for the two following reasons: as we are interested in obtaining the meniscus height over time with sufficient accuracy, we need to scale our entire system to a large resolution. A second numerical effect to consider is that, because of the finite width of the interface, the interface and the resulting fluid behavior can be overrepresented. To avoid this, the interface thickness should be small, as compared to the droplet radius GroSteRaa13 (). The droplet radius at a contact angle of is chosen to be , so that the interface thickness results in about of the droplet radius. It was found empirically that this drop size is sufficient to achieve reproducible results for the resulting hydrodynamics. All fluid volumes and system dimensions are kept constant and only the wall interaction parameters and a horizontal shift length, that brings the droplets into contact, are adjusted for all subsequent simulations of decreasing contact angles.

### 2.2 Initialization of coalescence

Both in experiment and in simulations, it is challenging to initiate coalescence and to define the time that marks the start of the coalescence. Here we provide technical details on how the simulations were performed.

A first problem is that the width of the diffuse interface and the fluid pressures are dependent on the fluid parameters, so that it is not possible to predict beforehand the correct densities at all positions. This is why equilibration during initialization is required. A lack of correct initialization will lead to strong artefacts, such as an enclosed bubble for droplets of a contact angle that can be avoided with careful initialization. To do so, we first equilibrate a horizontally centered single droplet at the wetting wall before a second drop is introduced.

The introduction of a second drop, and the initiation of coalescence is a subtle matter by itself. Here we shift the droplet to a system boundary with a full slip boundary condition. This effectively mirrors the droplet, as is depicted in the schematic figure 2. This is a magnified section of the system at the meniscus after shifting the droplet. Here, the effectively mirrored part is shown in slightly opaque and density profiles at different cross sections of the diffuse interface are sketched in Figs. 2 and 2. The mirrored part of the system shown in Fig. 2 does not need to be simulated, which reduces the simulation time. The density gradients shown in Fig. 2 of the two fluids exemplary show a transition from a majority of one fluid to the other, as for instance in the 1D cross section in Fig. 2, marked with ”Diffuse Interface”. This schematic representation of a diffuse interface identifies that the position of an according sharp interface is not clearly defined. Accordingly, the shift to the full slip boundary can be executed in different ways, like shown in Fig. 2. Here the schematic red density gradient stays in place, while the density gradient of the other droplet is shifted. The second gradient is drawn multiple times, transitioning from left to right.

To investigate the effect of the precise location of the second drop, we investigate the growth dynamics for different shifts, i.e. different initial positions. As an example a droplet with a contact angle of is moved by the default distance of lattice sites. The result is shown in figure 3, where the bridge height in time for different values of shift is recorded. As expected, overlapping droplets coalesce with an initial non-zero bridge height. By contrast, small separations between the drops cause a delay of the coalescence process by multiple timesteps. In this case diffusion occurs across the small separation of droplets, so that it takes some time before a detectable bridge has formed between the two drops. Further separation of the droplets causes the coalescence not to occur for several thousand timesteps. After timesteps all curves fall on a power law. In the inset of Fig. 3 it is shown that a collapse of the data can be achieved by manual shift of the time, which is a robust way to identify an appropriate definition of . This procedure will be followed for all plots in the remainder of the paper.

## 3 Results

t= | t= | t= | t= | t= |

t= | t= | t= | t= | t= |

In Fig. 4 we show snapshots of the coalescence process at the exemplary contact angles of and (as is the case in the experiments of EddWinSno13-2 ()). To represent the interface we use a bilinear interpolation of a threshold density which allows to obtain smooth data. The time series shows that a thin bridge appears between the two droplets, which grows both in height and width as time evolves. To quantify this evolution, we track the bridge height for a broad range of contact angles. This is shown in Fig. 5, where we show (scaled with the drop radius ) as a function of time (scaled with the inertio-capillarity time ). The closed symbols represent simulations for various contact angles. For contact angles below , the initial dynamics is consistent with a power law until the bridge becomes comparable to the drop size . This is perfectly in line with experiments. When the contact angle is , however, the slope of the data is smaller and suggests a smaller exponent, approaching the experimentally observed scaling. For a more detailed comparison, we include in Fig. 5 the data from EddWinSno13-2 (), which corresponds to experiments of water drops that coalesce in air. The experimental data shown here was shifted upwards, by a factor of , for the purpose of better visualization. However, even without this shift the experimental data lies about a factor above the numerical data. This quantitative difference can possibly be attributed to the fact that the simulations consider droplets that are immersed into an outer fluid of equal density. The transport inside the outer fluid does slow down the dynamics with respect to the case of drops in air, which is consistent with the observations in Fig. 5. Therefore a quantitative match of these is not to be expected, but in terms of scaling laws the simulations comply with experiments. As the wettability of the substrate alters the contact angle of the fluid, it alters the capillary pressure of the droplets. Due to the capillary pressure driving the coalescence, the contact angle alters the rate at which the meniscus grows. The representative scaling laws for this behavior, as well as the behavior of the fluid interface are discussed below.

### 3.1 Results for

To make further use of the simulation results, let us briefly revisit the usual scaling arguments for coalescence. The situation is best understood for contact angles , for which the horizontal scale and vertical scale are simply proportional to one another: the ratio of the two lengths is set by the tangent of the contact angle. This can for example be seen from Fig. 4, showing that the width of the meniscus increases as well as during the growth. Since sets the characteristic scale of the bridge, the capillary pressure can be estimated as

(4) |

Similarly, the inertial pressure is obtained as

(5) |

which then leads to the observed

(6) |

To further test the idea that the dynamics is governed by the growing length scale , one can attempt a collapse of the bridge profiles during the growth process. This is shown for the case in Fig. 6, where we overlay the meniscus shapes for different times, after rescaling the horizontal and vertical scales with . The scaled profiles indeed exhibit an excellent collapse. This confirms that the bridge growth is characterized by a universal spatial profile, and that the temporal dependence can be effectively absorbed in the growing length scale . The self-similarity only applies for the initial stages of coalescence, so the data shown are until the bridge height reaches about one third of the initial drop height. This limits the data to parts of the droplet deformed by the coalescence, where the scaling law is applicable. Small deviations far from the meniscus can be attributed to this effect. Figure 6 also shows the corresponding experimental plot from EddWinSno13-2 (), for which self-similarity was convincingly demonstrated as well. The numerical bridge shapes (for immersed drops) differ slightly from the experimental profiles, but the same principle of self-similarity is valid during the initial stages of coalescence.

Interestingly, the simulations allow one to extract information that is not easily accessible through experiments, such as the fluid velocities and . Inspired by the idea of self-similarity, we rescale the streamline patterns by again normalizing and by . The result is shown in Fig. 7, where the streamlines are obtained after scaling the velocities with (different times are visualized using different colors). The streamline patterns exhibit an excellent collapse. It can be seen that the coalescence causes a recirculating flow, with a vortex located to the right of the symmetry axis, driving the meniscus upwards. The necessary rescaling of the velocity vectors can be understood by considering . This implies that , as was indeed used in preparing Fig. 7.

### 3.2 Results for

Let us now turn to the case of droplets with , for which the interfaces are tangent when brought into contact. As a consequence of this geometry, the horizontal and vertical scales are no longer the same. We therefore introduce the width of the bridge , indicated in Fig. 1, as the horizontal scale that is much smaller than . The geometry is such that

(7) |

and subsequently, the scaling laws need to account for this disparity of horizontal and vertical scales. The usual argument is that the capillary pressure reads

(8) |

which can be balanced with the inertial pressure

(9) |

This leads to

(10) |

and explains why the meniscus growth differs from the 2/3 law observed for smaller contact angles (cf. Fig. 5).

Once more, we will test these scaling ideas by searching for self-similar dynamics, both for the bridge shape and for the velocity profiles. The first of these tests is provided in Fig. 8, where the bridge profiles for are rescaled with on the horizontal axis and with in the vertical direction. A collapse is indeed observed, confirming the necessity of taking different horizontal and vertical scales. In addition the numerical profiles exhibit a perfect agreement with the experimental results for the bridge shape EddWinSno13-2 (). Intriguingly, however, we have not been able to obtain a convincing self-similarity for the velocity fields for . Following the logic above, one would expect for the horizontal velocity , while for the vertical velocity . However, the best “collapse” was obtained by empirically scaling the velocities respectively as and , and the result is shown in Fig. 9. One again observes a recirculating flow that leads to the bridge growth, but the associated vortex structure is not perfectly self-similar. In particular, we note that the vortex appears to become smaller in time, after rescaling, suggesting that and are not the correct scales for the velocity field. The velocities of strongest amplitude lie underneath the meniscus and are nearly only vertical. Mass conservation in this case is achieved by enlarging the respective area in time. This means that the usual scaling arguments of equations 8 and 9 might actually be too simplistic. For example, the self-similar scaling of the meniscus profiles implies that the typical curvature scales as , and not as , as was assumed in (8). This would change the coalescence exponent from 1/2 to 2/5, which does not concur with simulations and previous experiments. This observation on the velocity field suggests that the pressure scaling (9) needs to be revised. The flow field is more intricate than the scaling argument allows to believe. Uncertainties in the definition of the scaling argument undermine this requirement. This would be an interesting topic for future work, for which a larger range of numerical data would be required to conclusively infer the relevant scaling laws. Droplets with a contact angle of only differ from freely suspended coalescing droplets by a minor amount of surface friction. Therefore the scaling argument for freely floating droplets might need to be revisited as well.

## 4 Conclusion

We simulated the coalescence of submerged droplets with different contact angles and compared our results to experimental data. Similar growth rates for the bridge height in time, equally dependent on the contact angle could be found in this case. Despite quantitative differences of the interface position of the fluid interface between experimental data of droplets in air and the simulation of submerged droplets, the same rescaling argument revealed a self similarity in time. Being able to use the same scaling arguments to scale the interface position of both the experimental droplets in air and the submerged simulated droplets shows the universality of the scaling argument. We applied this scaling law to the velocity field and, for droplets of a contact angle, revealed the underlying velocities that cause the coalescence and give reasons for the scaling of the amplitude of the velocities. For droplets of a contact angle we presented that the velocities causing the coalescence are more intricate than the scaling laws indicate. This shows that, though these scaling laws seem to work for the interface position, the underlying estimate for the relevant scaling for the velocity appears to be inconsistent with the internal flow structure. Clearly, our simulations show that the droplet internals are more complex than usually assumed. Our findings have implications for the design of devices in open microfluidics where different fluids are transported on chemically patterned substrates. Understanding the formation, transport and the coaleascence of droplets in particular is mandatory to optimize these devices and ascertain a reliable long-term functionality.

## Acknowledgment

This research was carried out under project number M61.2.12454b in the framework of the Research Program of the Materials innovation institute M2i (www.m2i.nl). We highly acknowledge Océ-Technologies B.V. for financial support and the Jülich Supercomputing Centre for the required computing time.

### Footnotes

- email: j.harting@fz-juelich.de
- email: j.harting@fz-juelich.de
- email: j.harting@fz-juelich.de

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